llm.ipynb

{
 "cells": [
  {
   "cell_type": "code",
   "execution_count": 8,
   "metadata": {},
   "outputs": [],
   "source": [
    "from transformers import AutoTokenizer\n",
    "from nltk.translate.bleu_score import sentence_bleu, SmoothingFunction\n",
    "\n",
    "#word_tokenize = AutoTokenizer.from_pretrained(\"suayptalha/DeepSeek-R1-Distill-Qwen-0.5B-CoMa\")\n",
    "word_tokenize = AutoTokenizer.from_pretrained(\"deepseek-ai/DeepSeek-R1-Distill-Qwen-1.5B\")\n",
    "\n",
    "def calcular_bleu(texto_gerado, texto_referencia):\n",
    "    referencia = [word_tokenize(texto_referencia).input_ids]\n",
    "    gerado = word_tokenize(texto_gerado).input_ids\n",
    "    smoothie = SmoothingFunction().method1  \n",
    "\n",
    "    return sentence_bleu(referencia, gerado, smoothing_function=smoothie)"
   ]
  },
  {
   "cell_type": "code",
   "execution_count": 1,
   "metadata": {},
   "outputs": [],
   "source": [
    "import requests\n",
    "\n",
    "def create_completion(prompt, max_tokens, temperature, top_p, top_k):\n",
    "\ttry:\n",
    "\t\tresponse = requests.post(\"http://localhost:1234/v1/completions\", json={\n",
    "\t\t\t\"model\": \"deepseek-r1-distill-qwen-1.5b@iq3_xxs\",\n",
    "\t\t\t\"prompt\": prompt,\n",
    "\t\t\t\"max_tokens\": int(max_tokens),\n",
    "\t\t\t\"temperature\": float(temperature),\n",
    "\t\t\t\"top_p\": float(top_p),\n",
    "\t\t\t\"top_k\": int(top_k),\n",
    "\t\t\t\"stream\": False\n",
    "\t\t})\n",
    "\t\tresponse.raise_for_status()  # Lança erro se o status HTTP for 4xx ou 5xx\n",
    "\t\tresult = response.json()\n",
    "\t\treturn result['choices'][0]['text']\n",
    "\texcept Exception as e:\n",
    "\t\tprint(\"Erro em create_completion:\")\n",
    "\t\tprint(f\"Prompt: {prompt[:15]}...\")\n",
    "\t\tprint(f\"Parâmetros: max_tokens={max_tokens}, temperature={temperature}, top_p={top_p}, top_k={top_k}\")\n",
    "\t\tprint(f\"Erro: {e}\")\n",
    "\t\texit"
   ]
  },
  {
   "cell_type": "code",
   "execution_count": 2,
   "metadata": {},
   "outputs": [],
   "source": [
    "from datasets import load_dataset\n",
    "ds_stream = load_dataset(\"ccdv/arxiv-summarization\", \"section\", split=\"test\", streaming=True)"
   ]
  },
  {
   "cell_type": "code",
   "execution_count": 3,
   "metadata": {},
   "outputs": [
    {
     "name": "stdout",
     "output_type": "stream",
     "text": [
      "done\n"
     ]
    }
   ],
   "source": [
    "import threading\n",
    "import random\n",
    "\n",
    "class SampleReservoir:\n",
    "    def __init__(self, stream, k=40, max_items=None):\n",
    "        self.stream = stream\n",
    "        self.k = k\n",
    "        self.max_items = max_items\n",
    "        self.reservoir = []\n",
    "        self.lock = threading.Lock()\n",
    "        self.done = False\n",
    "\n",
    "    def update(self):\n",
    "        # Algoritmo de amostragem de reservatório com proteção de acesso\n",
    "        for i, item in enumerate(self.stream):\n",
    "            if self.max_items is not None and i >= self.max_items:\n",
    "                break\n",
    "            with self.lock:\n",
    "                if i < self.k:\n",
    "                    self.reservoir.append(item)\n",
    "                else:\n",
    "                    j = random.randint(0, i)\n",
    "                    if j < self.k:\n",
    "                        self.reservoir[j] = item\n",
    "        self.done = True\n",
    "        print(\"done\")\n",
    "\n",
    "    def get_samples(self):\n",
    "        with self.lock:\n",
    "            # Retorna uma cópia do reservoir atual\n",
    "            return list(self.reservoir)\n",
    "\n",
    "# Inicializa o objeto do reservoir\n",
    "reservoir = SampleReservoir(ds_stream, k=5, max_items=5000)\n",
    "\n",
    "# Inicia a thread de atualização (em background)\n",
    "update_thread = threading.Thread(target=reservoir.update, daemon=True)\n",
    "update_thread.start()"
   ]
  },
  {
   "cell_type": "code",
   "execution_count": 9,
   "metadata": {},
   "outputs": [
    {
     "data": {
      "text/plain": [
       "[{'article': 'the signatures of the strong interactions in the quark - gluon matter were found in heavy ion collisions experiments  @xcite . \\n there are proposals  @xcite suggesting that color - magnetic monopoles contribution can explain this rather unexpected property . \\n these proposals inspired a number of publications devoted to the properties and possible roles of the monopoles in the quark - gluon phase  @xcite . \\n lattice gauge theory suggests a direct way to study fluctuations contributing to the euclidean space functional integral , in particular , the color - magnetic monopoles can be studied . in a number of papers \\n the evidence was found that the nonperturbative properties of the nonabelian gauge theories such as confinement , deconfining transition , chiral symmetry breaking , etc . \\n are closely related to the abelian monopoles defined in the maximally abelian gauge @xmath3  @xcite . \\n this was called a monopole dominance  @xcite . \\n the drawback of this approach to the monopole studies is that the definition is based on the choice of abelian gauge . \\n there are various arguments supporting the statement that the abelian monopoles found in the mag are important physical fluctuations surviving the cutoff removal : scaling of the monopole density at @xmath4 according to dimension @xmath5 for infrared @xmath6 cluster  @xcite ; abelian and monopole dominance for a number of infrared physics observables ( string tension  @xcite , chiral condensate  @xcite , hadron spectrum     @xcite ) ; monopoles in the mag are correlated with gauge invariant objects - instantons and calorons  @xcite . \\n it has been recently argued that the mag is a proper abelian gauge to find gauge invariant monopoles since thooft - polyakov monopoles can be identified in this gauge by the abelian flux , but this is not possible in other abelian gauges  @xcite . \\n most of these results were obtained for @xmath0 gluodynamics but then confirmed for @xmath7 theory and qcd  @xcite . \\n listed above properties of abelian monopoles survive the continuum limit and removal of the gribov copy effects . \\n it is worth noticing that removal of gribov copy effects changes numerical values of monopole characteristics quite substantially  @xcite .    in this paper \\n we are studying thermal monopoles . \\n it was shown in ref . \\n @xcite that thermal monopoles in minkowski space are associated with euclidean monopole trajectories wrapped around the temperature direction of the euclidean volume . \\n so the density of the monopoles in the minkowski space is given by the average of the absolute value of the monopole wrapping number . \\n in  @xcite another approach to study thermal monopole properties in the quark - gluon plasma phase based on the molecular dynamics algorithm was suggested and implemented . \\n the results for parameters of inter - monopole interaction were found in agreement with lattice results  @xcite . \\n first numerical investigations of the wrapping monopole trajectories were performed in @xmath0 yang - mills theory at high temperatures in refs . \\n @xcite and  @xcite . \\n a more systematic study of the thermal monopoles was performed in ref . \\n it was found in  @xcite that the density of monopoles is independent of the lattice spacing , as it should be for a physical quantity . the density  density spatial correlation functions were computed in  @xcite . \\n it was shown that there is a repulsive ( attractive ) interaction for a monopole \\n monopole ( monopole  antimonopole ) pairs , which at large distances might be described by a screened coulomb potential with a screening length of the order of @xmath8 fm . in ref . \\n @xcite it was proposed to associate the respective coupling constant with a magnetic coupling @xmath9 . in the paper \\n @xcite trajectories which wrap more than one time around the time direction were investigated . \\n it was shown that these trajectories contribute significantly to a total monopole density at @xmath10 slightly above @xmath1 . \\n it was also demonstrated that bose condensation of thermal monopoles , indicated by vanishing of the monopole chemical potential , happens at temperature very close to @xmath1 . however , the relaxation algorithm applied in  @xcite to fix the mag is a source of the systematic errors due to effects of gribov copies . \\n it is known since long ago that these effects are strong in the mag and results for gauge noninvariant observables can be substantially corrupted by inadequate gauge fixing  @xcite . for the density of magnetic currents at zero temperature \\n it might be as high as @xmath11 . \\n for nonzero temperature the effects of gribov copies were not investigated until recently . in a recent paper  @xcite this gap was partially closed . \\n it was shown that indeed gauge fixing with sa algorithm and @xmath12 gauge copies per configuration gives rise to the density of the thermal monopoles @xmath13 to @xmath14 lower ( depending on the temperature ) than values found in  @xcite . \\n large systematic effects due to effects of gribov copies found in ref . \\n @xcite imply that results obtained in earlier papers  @xcite for the density and other monopole properties can not be considered as quantitatively precise and need further independent verification . \\n the quantitatively precise determination of such parameters as monopole density , monopole coupling and others is necessary , in particular , to verify the conjecture  @xcite that the magnetic monopoles are weakly interacting ( in comparison with electrically charged fluctuations ) just above transition but become strongly interacting at high temperatures . in this paper \\n we use the same gauge fixing procedure as in refs . \\n @xcite to avoid systematic effects due to gribov copies . \\n the careful study of the finite volume and finite lattice spacing effects was made in @xcite . \\n we fix our spatial lattice size to @xmath15 which was shown in ref . \\n @xcite to be large enough to avoid finite volume effects . \\n we check finite lattice spacing effects comparing results obtained on lattices with @xmath16 and 6 at two temperatures . \\n let us emphasize that our studies are computationally much more demanding in comparison with studies undertaken in refs . \\n @xcite , since we produce @xmath12 gribov copies per configuration to avoid gribov copies effect . for this reason \\n our check of the continuum limit is not as extensive as it was in refs . \\n @xcite . \\n the important contribution of this work to the thermal monopole studies is a check of universality . in studies of magnetic currents at zero temperature it was found  @xcite that the density of the infrared magnetic currents is different for different lattice actions with difference as large as @xmath14 . \\n the conclusion was made that the ultraviolet fluctuations contribute to the infrared density and this contribution has to be removed . \\n partial removal was made by the use of the improved action . in present paper \\n we use the improved lattice action - tadpole improved symanzik action and compare our results for the density and other quantities with results obtained with the wilson action  @xcite . \\n we find that the universality holds for monopoles which do not form short range ( ultraviolet ) dipoles . \\n we also want to point out that in this work we use more natural procedure of computing monopole correlators in comparison with papers  @xcite and  @xcite . \\n it was mentioned in ref . \\n @xcite that monopole trajectories had a lot of small loops attached to them which were uv noise . \\n presence of such loops do not allow to determined monopole spatial coordinates unambiguously for all time slices . \\n this problem was bypassed in  @xcite by using only one time slice . \\n we remove the small loops attached to thermal monopole trajectories and thus we are able to determine the monopole coordinates in every time slice unambiguously . \\n then we use all time slices to compute the correlators what allows us to decrease the statistical errors substantially . \\n we studied the @xmath0 lattice gauge theory with the tadpole improved symanzik action :          parameter @xmath22 is the input tadpole improvement factor taken here equal to the fourth root of the average plaquette p = @xmath23 . \\n we use the same code to generate configurations of the lattice gauge field as was used in ref . \\n our calculations were performed on the asymmetric lattices with lattice volume @xmath24 , where @xmath25 is the number of sites in the time ( space ) direction . \\n the temperature @xmath10 is given by :      where @xmath27 is the lattice spacing . to determine the values of @xmath22 we used results of ref . \\n @xcite either directly or to make interpolation to necessary values of @xmath28 . \\n the critical value of the coupling constant for @xmath29 is @xmath30 @xcite . \\n for @xmath29 the ratio @xmath31 was obtained using data for the string tension from ref . \\n @xcite again either directly or via interpolation . for @xmath32 ratio @xmath31 \\n was taken to be equal to the ratio for @xmath29 multiplied by factor @xmath33 . in  table \\n [ tab : lattice_size ] we provide the information about the gauge field ensembles and parameters used in our study . \\n we apply the simulated annealing ( sa ) algorithm which proved to be very efficient for this gauge  @xcite as well as for other gauges such as center gauges  @xcite and landau gauge  @xcite . to further decrease the gribov copy effects we generated @xmath12 gribov copies per configuration starting every time gauge fixing procedure from a randomly selected gauge copy of the original monte carlo configuration .',\n",
       "  'abstract': 'the properties of the thermal abelian color - magnetic monopoles in the maximally abelian gauge are studied in the deconfinement phase of the lattice @xmath0 gluodynamics . to check universality of the monopole properties we employ the tadpole improved symanzik action . \\n the simulated annealing algorithm combined with multiple gauge copies is applied for fixing the maximally abelian gauge to avoid effects of gribov copies . \\n we compute the density , interaction parameters , thermal mass and chemical potential of the thermal abelian monopoles in the temperature range between @xmath1 and @xmath2 . in comparison with earlier findings our results for these quantities \\n are improved either with respect to effects of gribov copies or with respect to lattice artifacts .'},\n",
       " {'article': 'recently , we described a method to perform quantum monte carlo ( qmc ) calculations for lattice fermions @xcite . \\n we introduced an effective hamiltonian , by which the sign problem that is usually encountered in such systems , can be avoided . \\n we proved that it leads to an upper bound for the ground - state energy . \\n this fixed - node monte carlo ( fnmc ) method for lattice systems is very much inspired by the similar method , developed by ceperley _ \\n @xcite , for continuous systems .    in this paper \\n we want to show that , in analogy to the method for continuum problems , it is possible to extend the fnmc method for lattice systems in order to obtain approximate information about the true ground state of the system . \\n nodal relaxation _ method , as it is called by ceperley _ \\n @xcite , can be straighforwardly implemented also on lattice systems . \\n we will give a formalism for this method , using the ( theoretical ) results of the fnmc method described in @xcite . \\n also , we will give a few more examples of applications of these methods , in comparing our results to those presented by other authors , for a few systems frequently used in the literature . \\n in the next section we will recall the basic formulas of the green function monte carlo ( gfmc ) formalism , and give our notation and interpretation of the concept of importance sampling . \\n after a few summarizing remarks on the fixed - node monte carlo method , we will show in section  [ sec - power ] how the results of this method can be used to calculate properties of the true ground state of the system . in section  [ sec - applications ] \\n we present a few examples of applications of both methods , and we conclude this paper by a discussion on the applicability of the methods and the need for further investigation of possible wave functions .    a much more elaborate explanation and discussion of the fnmc method and the extended method , information on the implementation of both methods , and some more examples of applications , have been given in refs . and . \\n the gfmc method , as we use it , is based on the _ projection _ operator @xmath0 by which the ground state of the hamiltonian @xmath1 is filtered from a trial state @xmath2 , which is known or can be calculated for each configuration @xmath3 in the configuration space @xmath4 . \\n the parameters @xmath5 and @xmath6 are to be chosen appropriately . after applying this operator @xmath7 times , \\n an approximation @xmath8 of the ground state is obtained , which closely resembles the ground state for large @xmath7 . \\n the energy of this state can be formally calculated as @xmath9 \\\\langle      r_0|\\\\psi_{\\\\text{t}}\\\\rangle } { \\\\sum_{{\\\\cal          r}}\\\\langle\\\\psi_{\\\\text{t}}| r_{n}\\\\rangle \\\\left[\\\\prod_{i=1}^{n }      \\\\langle r_{i}|f|r_{i-1}\\\\rangle\\\\right ] \\\\langle      r_0|\\\\psi_{\\\\text{t}}\\\\rangle } , \\\\label{mixedestimate}\\\\end{aligned}\\\\ ] ] where @xmath10 is a path in the configuration space . as we will see in the actual implementation of this calculation \\n , the wave function has to be known in the end point of each path , and therefore @xmath11 must be used in this expression in stead of @xmath12 . \\n this is called a _ mixed estimate _ of the energy . \\n the expression  ( [ mixedestimate ] ) can usually not be calculated exactly . in the monte carlo scheme , \\n only a limited number of paths @xmath13 is used for the calculation of this expression . \\n we can rewrite  ( [ mixedestimate ] ) as @xmath14 where @xmath15 is the _ local energy _ in the configuration @xmath3 . \\n the quantity @xmath16 can be interpreted as the probability of choosing a complete path @xmath13 , and each path carries a _ weight _ or _ multiplicity _ @xmath17 . \\n if one makes sure that @xmath18 and @xmath19 satisfy @xmath20\\\\langle r_0|\\\\psi_{\\\\text{t}}\\\\rangle , \\\\ ] ] the energy @xmath21 can be calculated as @xmath22 where the summation is now restricted to some number of paths , chosen according to the probability @xmath16 . in the limit of using infinitely many paths , \\n this calculation becomes exact ; in case of a finite number of paths , a statistical error bar can be defined .    in the definition of @xmath18 and @xmath19 \\n one can include ways to make the sampling of the wave function more efficient . \\n this is called _ importance sampling _ , and usually refers to the idea that one should try to sample more often in regions where the trial wave function has a large absolute value . \\n we give a description which includes the possibility of performing importance sampling by means of a guiding function @xmath23 . \\n this function must be positive everywhere ; often , it is taken to be the absolute value of the trial wave function . \\n we denote the probability for choosing a path as @xmath24 here , the probability for the first configuration of the path to be @xmath3 is @xmath25 and the probability of each subsequent step of the path is defined by @xmath26 when using this probability for the paths , one has to take @xmath19 as @xmath27 \\\\frac{\\\\langle\\\\psi_{\\\\text{t}}|r_{n}\\\\rangle}{\\\\langle\\\\psi_{\\\\text{g}}|r_{n}\\\\rangle }      , \\\\ ] ] where the weight factors @xmath28 can be calculated for each step @xmath29 separately as @xmath30 these relations basically define the monte carlo procedure . additionally , one can make use of _ branching _ \\n @xcite , to avoid that the variance of the calculated result increases too rapidly .    in the monte carlo scheme \\n , one can thus choose the starting configurations of the paths according to @xmath31 , and each subsequent configuration according to the _ stochastic matrix _ defined by @xmath32 . interpreting the paths as random walks in the configuration space , one usually calls the configurations chosen _ walkers_. in our interpretation , the starting set of walkers that one uses in the monte carlo calculations is distributed according to the square of the trial wave function . \\n one can calculate how the walkers are redistributed after @xmath7 steps , considering also the weight they carry : @xmath33 this expression can be easily evaluated using the relation  ( [ pmrelation ] ) for @xmath18 and @xmath19 : @xmath34\\\\langle r_0|\\\\psi_{\\\\text{t}}\\\\rangle\\\\\\\\ &    = & \\\\langle\\\\psi_{\\\\text{t}}|r\\\\rangle\\\\langle r|{\\\\cal      f}^{n}|\\\\psi_{\\\\text{t}}\\\\rangle \\\\\\\\ & = &    \\\\langle\\\\psi_{\\\\text{t}}|r\\\\rangle\\\\langle r|\\\\psi^{(n)}\\\\rangle . \\n \\\\label{walkersdistribution}\\\\end{aligned}\\\\ ] ] thus , after a sufficiently large number of steps the walkers are distributed according to the product of the trial wave function and the ground - state wave function of the hamiltonian considered . \\n the fixed - node monte carlo method uses in fact the same formalism as the general green function monte carlo , presented in the previous section , but with a modified hamiltonian @xmath35 to avoid steps that could introduce a change of sign in the weights or the probabilities ( the _ sign problem_@xcite ) . the gfmc procedure is straightforwardly applied to this _ effective _ hamiltonian , for which a prescription has been given in refs . and . \\n thus , by the fnmc method , information is obtained not on the ground state of the hamiltonian @xmath36 one is interested in , but on the ground state of @xmath35 . \\n it has been proven that the ground - state energy of @xmath35 provides an upper bound for the ground - state energy of @xmath36 . of course \\n , it would be better to obtain information directly on @xmath36 . \\n as we will see , under certain circumstances this is possible , using the fnmc result as input for a new calculation , called _ \\n nodal relaxation_. it strongly resembles the method described by ceperley and alder @xcite for a continuum problem . \\n the method suffers from the sign problem , but it may yield convergent results before the fluctuations destroy the accuracy of the calculations . \\n let us rewrite the expression  ( [ walkersdistribution ] ) to give the distribution of the configurations in the fnmc procedure after @xmath7 steps : @xmath37 where @xmath38 is supposed to be a good approximation of the ground state @xmath39 of @xmath40 . \\n the idea is now that @xmath39 is sufficiently close to the ground state @xmath41 of @xmath36 , such that in gfmc procedure used on @xmath36 convergence can be obtained within a relatively small number of steps . \\n thus , we modify  ( [ psigfmc ] ) in the following way : @xmath42 then , we also have to modify the expression  ( [ mixedestimate ] ) for the mixed estimate of the energy : @xmath43 \\\\langle      r_0|\\\\psi_{\\\\text{eff}}\\\\rangle } { \\\\sum_{{\\\\cal          r}}\\\\langle\\\\psi_{\\\\text{t}}| r_{n}\\\\rangle \\\\left[\\\\prod_{i=1}^{n }      \\\\langle r_{i}|f|r_{i-1}\\\\rangle\\\\right ] \\\\langle      r_0|\\\\psi_{\\\\text{eff}}\\\\rangle } .\\\\end{aligned}\\\\ ] ] note that we still have to put @xmath11 in this expression , as that is the only available information we have in each configuration \\n . however , in the starting configurations of the paths , the trial wave function has been replaced by the effective ground - state wave function , of which we have information through the distribution of the walkers in the fnmc procedure . \\n we have to pay further attention to the fact that sign changes can now occur , which have to be embedded in the transition probabilities and multiplicities . \\n we can use the following guiding procedure , adapted from the regular gfmc scheme described in the previous section : the probability to start in a configuration @xmath3 is given by the fixed - node resulting distribution : @xmath44 the transition probabilities are given by @xmath45 with the modified weight factor @xmath46 the absolute value has to be taken to make sure that the transition probabilities remain positive , such that the procedure can still be interpreted as a stochastic walk . with these expressions replacing  ( [ startingprob ] ) , \\n ( [ hoppingprob ] ) , and  ( [ hoppingmult ] ) , the equations  ( [ guidingprobability ] ) and  ( [ guidingweight ] ) can again be used for the total probability and the total `` weight \\'\\' of a path , respectively . \\n note that the weights can now be negative , due to the possibly different signs of the wave function in the starting and end configurations of the path .    by this formalism \\n , one can thus try to obtain information directly on the true ground state of the hamiltonian , using the fixed - node result as a starting point . in the following section \\n , we will show a few examples of applications of this method . \\n first , we visualize how the fnmc and the nodal - relaxation method work for the hubbard model on a small system , the 2 @xmath47 2 @xmath47 2 cube , with @xmath48 . \\n we have performed exact calculations for this system@xcite , in order to be able to compare the monte carlo results and check whether the program has been correctly implemented . in figures \\n [ fig1 ] and  [ fig2 ] , we show calculations for this system at half filling and with zero total spin in the @xmath49-direction . in figure  [ fig1 ] , the first 250 steps in the fixed - node monte carlo calculation , using a homogeneous mean - field wave function as trial wave function , \\n are shown . as can be seen , after some 100 steps the energy measured starts fluctuating around the exact ground - state energy of the effective hamiltonian ( indicated by the drawn line ) . \\n the square at the right indicates the energy that one obtaines after averaging over several thousands of steps ( not shown in this figure ) , with a statistical error which is smaller than the symbol size . in figure \\n [ fig2 ] , two separate calculations of nodal relaxation are shown ; one using the same trial wave function as in figure  [ fig1 ] ( indicated by h ) , the other using a mean - field wave function with antiferromagnetic ordering imposed on the spins ( indicated by af ) . \\n the horizontal lines indicate the exact ground - state energies of the effective ( fn ) hamiltonians using the h and the af trial functions , respectively , and of the true hamiltonian . \\n the resulting energy after each step is indicated by an error bar ( the energy measured being the middle value of the error bar ) . \\n as can be seen , the size of the error bars in both calculations first decreases with increasing number of steps , and then starts increasing , indicating the existence of the sign problem . \\n the calculation marked h seems to converge to the correct value before the sign problem arises ; the af calculation does not has not converged at that point . \\n clearly , this is due to the fact that the fixed - node energy found when using the af wave function is significantly higher than the resulting energy in the other fixed - node calculation . \\n this nicely demonstrates that the exact result can be reached , but only if the fixed - node result is close enough to the true ground state . \\n we have performed some more calculations for the hubbard model . in table \\n [ tab1 ] , we compare results of calculations of the ground - state energy for a 4 @xmath47 4 square with periodic boundary conditions ( pbc ) , with 5 spins up and 5 down , and @xmath50 . for this system , \\n exact and approximate results are available in the literature . \\n as can be seen , in the case of @xmath50 , the fixed - node method yields an upper bound for the ground - state energy which is quite close to the exact value , and nodal relaxation leads to the exact result with an error bar of only 0.05% . in table \\n [ tab2 ] , we show the results of various calculations of the ground - state energy in a 10 @xmath47 10 system ( pbc ) , at half filling and with zero total spin in the @xmath49-direction , also for @xmath50 \\n . there are no exact results available for this system , but several results of mean - field and quantum monte carlo calculations can be found in the literature . as can be seen , \\n our results are in very good agreement with previous qmc results by hirsch @xcite and white _ et al._@xcite . \\n first we would like to make a few additional remarks on the calculations we have performed . as one can see from table  [ tab1 ] , adding a gutzwiller factor to the bare mean - field wave function greatly improves the ( variational ) energy obtained from the mean - field calculation . in the fixed - node calculation , however , the energy is hardly improved by adding the gutzwiller factor to the trial wave function . \\n considering also other calculations we performed , we feel that this is a rather general feature of the fixed - node method . in the fixed - node method , \\n the energy that is obtained is determined by the _ sign structure _ of the trial wave function , via the ratios of the wave function in neighboring configurations with different signs . in \\n order to significantly improve the energy , one must be able to change the sign of the trial wave function in individual configurations , as that is the most important factor determining the energy that can be obtained . by a gutzwiller factor ( or , similarly , a jastrow factor ) one does not change the sign , but only the ratios of the wave function . \\n another interesting point is that the monte carlo calculations become less stable for larger @xmath51 . \\n this is due to the fact that the parameter @xmath5 has to be taken smaller in that case , such that convergence is slowed down . for the fixed - node method \\n this is not a very big problem , as one can simply sample for a longer time to obtain a result with desired accuracy , but in the nodal - relaxation method one can not afford to have longer paths in the calculations , as the sign problem starts showing up after a certain number of steps . \\n another problem concerns the observables that can be calculated . for operators that commute with the hamiltonian , similar formulas as have been given for the energy in section  [ sec - gfmc ] can be used , although ( in fixed node ) the results obtained for operators other than the hamiltonian itself can not present a bound to the exact result . for operators that do not commute with the hamiltonian , however , there is a more serious problem ; in that case , the mixed estimate does not yield the correct value of the observable for the ground state of the ( effective or true , depending on the method ) hamiltonian . \\n usually , one uses an _ extrapolated estimate_@xcite in that case , taking two times the mixed estimate minus the variational result ( i.e. , the value of the observable in the trial state ) . in practice , this leads to rather good results ; however , one is unable to check how good the approximation is . \\n recently , zhang _ et al._@xcite presented the _ constrained path monte carlo _ \\n method for lattice fermions , which they claim to be a better method than fixed node . \\n like we , they apply some kind of fixed - node principle , but in a _ continuous _ space of slater determinants , which seems to cause that the cpmc energy is a better approximation of the true energy than the fixed - node energy . also , they claim that they have a better method ( _ backtracing _ ) to perform calculations for non - commuting operators . \\n it is not very clear to us how cpmc compares to fixed node combined with nodal relaxation . \\n it seems to us that our method is more generally applicable , as we can use any wave function as trial wave function ( as long as it can be calculated relatively easily ) and we can also treat systems of frustrated bosons or spins , while their method restricts the trial wave function to be a slater determinant . in any case , it would be very interesting to make a better comparison of both methods for some different systems . \\n finally , we state that the most important ingredient of our method is the trial wave function . \\n the quality of the trial function , i.e. , its sign structure , determines how good the approximation is that can be obtained . \\n this is not a trivial problem , for , as ceperley states , `  little progress [ has been made ] in stating exact conditions that nodes must obey . \\' \\n @xcite most studies of wave functions aim at improving the energy of the wave function itself , while for our purposes it would be necessary to explore its sign structure , in order the improve the energy that results after a fixed - node monte carlo simulation . \\n we still not have a clear understanding , yet , of the requirements that a wave function must fulfill to make a good fixed - node trial wave function . \\n however , we feel that the fixed - node method combined with nodal relaxation offers great new opportunities to tackle problems of lattice hamiltonians . \\n this work is part of the research program of the stichting voor fundamenteel onderzoek der materie ( fom ) , which is financially supported by the nederlandse organisatie voor wetenschappelijk onderzoek ( nwo ) . \\n van bemmel , d.f.b . \\n ten haaf , w. van saarloos , j.m.j . \\n van leeuwen , and g. an , phys . \\n lett . * 72 * , 2442 ( 1994 ) . \\n ten haaf , h.j.m . \\n van bemmel , j.m.j . \\n van leeuwen , w. van saarloos , and d.m . \\n ceperley , phys . \\n b * 51 * , 13039 ( 1995 ) . \\n d.m . ceperley and b.j . \\n alder , phys . \\n . lett . * 45 * , 566 ( 1980 ) ; science * 231 * , 555 ( 1986 ) . \\n anderson , j. chem . \\n phys . * 63 * , 1499 ( 1975 ) ; * 65 * , 4121 ( 1976 ) . \\n d.m . ceperley and b.j . \\n alder , j. chem . \\n * 81 * , 5833 ( 1984 ) . \\n ten haaf , _ on the magnetic phase diagram of the hubbard model _ , thesis , university of leiden , 1995 . \\n van bemmel , _ real - space aspects of correlated fermions _ , thesis , university of leiden , 1995 . n. trivedi and d.m . \\n ceperley , phys . rev . \\n b * 40 * , 2737 ( 1989 ) ; * 41 * , 4552 ( 1990 ) . \\n see , e.g. , the following papers : h. de raedt and w. von der linden , _ quantum lattice problems _ , in _ topics in applied physics _ , \\n vol .  71 : \\n _ the monte carlo method in condensed matter physics _ , edited by k. binder ( springer - verlag , berlin , 1992 ) ; s. sorella , s. baroni , r. car , and m. parrinello , europhys \\n * 8 * , 663 ( 1986 ) ; e.y . loh , jr . \\n gubernatis , r.t . \\n scalettar , s.r . \\n white , d.j . \\n scalapino , and r.l . \\n sugar , phys . rev . \\n b * 41 * , 9301 ( 1990 ) ; s. fahy and d.r . \\n hamann , phys . \\n b * 43 * , 765 ( 1991 ) ; m. boninsegni and e. manousakis , phys . rev . \\n b * 46 * , 560 ( 1992 ) ; m. suzuki , physica a * 194 * , 432 ( 1993 ) . \\n the exact results have been obtained by means of numerical diagonalization routines . \\n group theory was used to reduce the matrix to blocks of @xmath52 or smaller . \\n see also j. callaway , d.p . \\n chen , and y. zhang , phys . \\n b * 36 * , 2084 ( 1987 ) . \\n s. zhang , j. carlson , and j.e . \\n gubernatis , phys . \\n * 74 * , 3652 ( 1995 ) . \\n a. parola , s. sorella , s. baroni , r. car , m. parrinello , and e. tosatti , physica c * 162 - 164 * , 771 ( 1989 ) . \\n denteneer and m. blaauboer , j. phys . : condens . \\n matter * 7 * , 151 ( 1995 ) . \\n hirsch , phys . \\n b * 31 * , 4403 ( 1985 ) . \\n white , d.j . \\n scalapino , r.l . \\n sugar , e.y . \\n loh , j.e . \\n gubernatis , and r.t . \\n scalettar , phys . rev . \\n b * 40 * , 506 ( 1989 ) . \\n d.m . ceperley and m.h . \\n kalos , in _ topics in current physics _ , vol .  7 : _ monte carlo methods in statistical physics _ , edited by k. binder ( springer - verlag , berlin , 1979 ) ; k.e . \\n schmitt and m.h . \\n kalos , in _ topics in current physics _ , vol . \\n 36 : _ applications of the monte carlo method in statistical physics _ , edited by k. binder ( springer - verlag , berlin , 1984 ) . \\n ceperley , j. stat . \\n phys . * 63 * , 1237 ( 1991 ) . \\n .[tab1 ] comparison of the exact ground - state energy to the energy of mean - field and gutzwiller wave functions , and to the energy obtained by mc simulations , for the 4 @xmath47 4 square ( pbc ) , with 5 spins up and 5 down , for @xmath50 . a mean - field ( mf ) homogeneous ( h ) \\n wave function has been used . \\n the gutzwiller wave function ( gmf ) was used with @xmath53 ; its energy was calculated by variational monte carlo . for the fixed - node ( fn ) and nodal relaxation ( nr ) monte carlo calculations , \\n a trial wave function has been used as indicated . \\n energies are given per site and in units of @xmath54 . \\n constrained path monte carlo ( cpmc ) results were taken from ref . , exact results from ref .. [ cols=\"^,^,^,^,^,^,^,^\",options=\"header \" , ]',\n",
       "  'abstract': 'in a previous paper , we have described a method to perform fixed - node quantum monte carlo calculations for lattice fermions . in this paper , we present an extension of this method , by which it is possible to find information on the properties of the exact ground - state wave function . \\n we give some further illustrations of the fnmc and the extended methods .'},\n",
       " {'article': 'catalogs of galaxy clusters with a large range of redshifts and cluster x - ray luminosities are an ideal basis for the test of cosmological parameters ( e.g. henry 2000  ; borgani et al . \\n 2001 ) and the study of cluster formation and evolution . \\n the bright and southern serendipitous high redshift archival rosat cluster ( sharc ) surveys provide a sample of clusters detected in rosat observations over two decades of x - ray luminosities ( 10@xmath2 l@xmath3erg / s ) with redshifts between 0.2 and 0.8 ( romer et al . 2000  ; collins et al . 1997  ; burke et al . \\n 1997 ) . \\n we present here preliminary results based on the follow - up observations of three of these selected galaxy clusters with xmm \\n newton  : rx  j0256.5 + 0006 , rx  j2237.0 - 1516 and rx  j1200.8 - 0328 . for the first time \\n , the new generation of x - ray observatory , like xmm - newton and _ chandra _ give capabilities to do precise spectroscopic and imaging analysis at the same time ( see e.g arnaud et al . \\n 2002a ) . \\n our analysis is based on the three epic cameras , mos1&2 and pn . throughout the paper , \\n we use a cosmology with h@xmath4km / s / mpc , @xmath5 and @xmath6 . \\n the error bars are given with a confidence level of 90% . \\n all the data presented here are treated with the version 5.2 of the sas ( science analysis software ) . \\n we select event patterns and time intervals of low background as described in majerowicz et al . \\n table 1 shows the effective exposure time of our observations after flare rejection . \\n this suggests that this cluster does not host a strong cooling flow . \\n this was already seen in rx  j1120.1 + 4318 , a relaxed cluster at z=0.6 ( arnaud et al . \\n 2002a ) also found in the sharc survey . \\n the global temperature for this cluster is 5.1@xmath1kev . \\n its surface brightness profile is fitted by a @xmath7-model and the parameters are  : @xmath7=0.64 and @xmath80.51@xmath9228kpc . \\n arnaud , m. , neumann , d.m . , \\n aghanim , n. , et al , 2001 , , 365 , l80 arnaud , m. , majerowicz , s. , lumb , d. , et al , 2002a ,  in press , astro - ph/0204306 arnaud , m. , 2002b , this issue borgani , s. , rosati , p. , tozzi , p. , et al , 2001 , , 561 , 13 burke , d.j . , collins , c.a . , \\n sharples , r.m . , et al , 1997 , , 488 , l83 collins , c.a . , \\n burke , d.j . , \\n romer , a.k . \\n , et al , 1997 , , 479 , l117 henry , j.p . , \\n 2000 , apj , 534 , 565 lumb , d. , 2002 , xmm - soc - cal - tn-0016 majerowicz , s. , neumann , d.m . & reiprich , t.h . , 2002 , \\n submitted to , astro - ph/0202347 neumann , d.m . \\n & bhringer , h. 1997 , , 289 , 123 roettiger , k. , loken , c. & burns , j.o . , 1997 , , 109 , 307 romer , a.k . , nichol , r.c . , \\n holden , b.p . \\n , et al , 2000 , , 126 , 209 schindler , s. & mller , e. , 1993 , , 272 , 137 snowden , s.l . , egger , r. , freyberg , m.j . \\n , et al , 1997 , , 485 , 125 takizawa , m. , 1999 , , 520 , 514',\n",
       "  'abstract': 'we present the follow - up of three medium redshift galaxy clusters from the sharc survey observed with xmm  newton . \\n we studied rx  j0256.5 + 0006 which shows two components which are very likely in interaction . \\n the smallest component exhibits a comet - like structure indicating ram pressure stripping as it falls onto the main cluster . the second cluster , rx  j2237.0 - 1516 is an elliptical cluster with a gas temperature of [email protected] . the third cluster , rx  j1200.8 - 0328 seems to be in a relaxed state because its shape is regular and we do not see obvious temperature gradient . \\n its mean temperature is 5.1@xmath1kev . \\n # 1_#1 _ # 1_#1 _ =    # 1 1.25 in .125 in .25 in'},\n",
       " {'article': 'molecular nanostructures , where each individual molecule has its own function are emerging materials for the next generation of electronic devices and components . due to the increasing success in fabrication of self - assembled molecular monolayers ( sam ) and advancement of experimental techniques at one hand , as well as the development of powerful computational facilities for material science simulations on the other , \\n various classes of molecules have been investigated and proved to be promising candidates for future applications @xcite , and references therein . \\n ever since the conductance of a molecular junction was experimentally quantified in the mechanically controllable break - junction experiments with benzene 1,4-dithiol sams onto golden electrodes @xcite , benzene - based molecules , also the subject of the present study , have been intensively investigated . \\n nonlinearity , negative differential resistance , conductance switching , found in various benzene derivatives are some of the many interesting properties that make these systems attractive for investigation from both , experimental and theoretical point of view @xcite . \\n mechanisms underlying the electron transport in these systems , which are predominated by the quantum - mechanical effects are complex and still a matter of debate . in this respect , theoretical studies and models are crucial for rationalizing the existing experimental data , and even more , for proposing new candidate systems and guiding the fabrication of electronic components .    in the focus of our interest is a class of anthracene based organic molecules containing flexible side groups , denoted as rotor - stator molecular systems @xcite . so far , molecular junctions involving anthracene molecules have been extensively investigated . \\n controllable break junction experiments show that anthracene molecules could be considered as highly conductive single molecule elements , due to direct @xmath0-binding of the molecular orbitals to golden electrodes @xcite . \\n also , clear signatures for the formation of conducting hybrid junctions composed of single anthracene molecules , connected to chains of platinum atoms were recorded by break junction technique in @xcite . \\n this opens the ways towards fabrication and realization of anthracene based molecular electronic components .    despite of the vast amount of papers dedicated to \\n linear anthracene molecules , studies that are dealing with species containing side groups are lacking . as it was experimentally confirmed that the molecular conductance does not only depend on the chemical properties of the molecule , but it is the conformation that might have a substantial impact on the charge transport @xcite , it should be expected that the presence of side groups in the aromatic compounds will allow some new functions of the future molecular electronic devices . \\n the system we investigate here was proposed in our previous work as a single - molecule switching component , built of anthracene containing aldehyde side group bound to the central benzene ring . \\n we showed that due to the presence of a flexible dipolar aldehyde group , this could act as a bistable rotor - stator system . \\n depending on the orientation of the side aldehyde group with respect to the three static benzene rings , this system could be found in a stable state , denoted as planar conformer further on , and a metastable state ( the top of the double well ) , when the side group is oriented perpendicularly to the stator part , denoted as perpendicular conformer . applying the non - equilibrium green s function formalism ( negf ) , we studied the current - voltage ( @xmath1 ) curves in the coherent transport regime , simulating a metal - molecule - metal junction , including also the gating field effects @xcite . \\n conformational dependence of the transport properties of such a system was evident , since two distinguishable @xmath1 curves for the two respective conformers were obtained . \\n in @xcite we also paid a special attention on the possibilities to control the intramolecular torsional dynamics by application of external electric field in the proposed molecule . \\n we also showed that bistability of this system could be controlled and fine tuned by an external electric field , even under realistic conditions , reporting also the temperature dependence of transition probabilities and lifetimes . \\n the previously obtained results , especially the controllability of this molecular device are of crucial importance for further investigations , since stability and control of single - molecule electronic devices is one of the main limitations for operability of the prospective electronic devices at room temperatures . \\n transport regime via a metal - molecule - metal junction is in principle dictated by the position of the molecular charge carrying orbitals and electrodes fermi level @xcite . \\n motivated from the most recent findings , regarding the electron tunneling in linear aromatic compounds , showing that there is a gap between the molecular charge carrying orbital and the fermi level of the metallic electrodes @xcite , in the present study we are focused on the electron transmission via anthracene aldehyde molecular barrier in the tunneling transport regime . when the molecular charge carrying orbital is above the electrodes fermi level , than the electron transmission in the metal - molecule - metal junction is seen as tunneling via an insulating barrier . \\n recently , experimental observations @xcite showed that quasiclassical ( wkb ) approach gives successful interpretation of the tunneling currents through a molecular insulating barrier and the obtained results fit well with the simmons formula @xcite . \\n we adopt this methodology for the purposes of our analysis , combining it with accurate electronic structure calculations from first principles . \\n to evaluate the transmission coefficients and tunneling current within the wkb approach , we consider model barriers , encompassing two distinct cases , first neglecting the effects of the molecular internal structure in the transmission process - the case of simple rectangular barrier , and second , we account for these effects via the sinusoidal position dependence of the barrier . \\n we pay special attention of the conformational effects , calculating the current - voltage curves for various orientations of the aldehyde group with respect to the stator part . in the present work \\n we also improve our single molecule analysis , including the end dithiol bonds , that are usually used in fabrication of metal - molecule - metal junctions .    the obtained results for the transmission via the studied molecular segment suggest that molecular internal structure , incorporated in the position dependence of the tunneling barrier along the molecular bridge can not be neglected under realistic conditions . conformational dependence of the barrier height and thus , the tunneling current confirms that molecular geometry plays crucial role in the electron transport , allowing bistability and enhancing the electronic properties with respect to pure anthracene . \\n taking into account the recent interest in aromatic compounds , we believe that the proposed model to study tunneling of electrons via molecular interfaces containing side groups , that is complementary to our previous analysis of the coherent transport regime contributes to the modeling and predicting the behavior of newly proposed molecular species , and consequently designing adequate experiments .    the paper is organized as follows : in section ii we introduce our model , in section iii we give an overview of the methodology and computational details , in section iv results and discussion are presented and section v comprises our conclusions . \\n we consider a model that describes tunneling of electrons in rotor - stator molecular interfaces , incorporating accurate _ ab initio _ \\n data for anthracene aldehyde molecular species . \\n the model is developed within the frameworks of the wkb approximation , which is valid for barriers having width of the order of 10 angstroms at heights of the order of several ev , applicable in our case @xcite . \\n when one wants to calculate the transmission probability within the wkb approximation , the main problem is to introduce a realistically shaped potential barrier . \\n it is a quite complex task to determine the actual height of the tunneling barrier , taking into account various factors that affect the electronic structure of the molecule when bound to electrodes out of equilibrium . \\n also the properties of the environment have their impact on the energetic barrier by which the tunneling of electrons in metal - molecule - metal junctions is governed . \\n the simplest , but yet sufficient approach to capture at least the qualitative picture is to consider a rectangular barrier having a height that equals the difference between the fermi level of the metal and the charge carrying orbital ( homo for holes and lumo for electrons ) . \\n since we are considering here a newly proposed anthracene based molecular species , we rely on recent results regarding electron tunneling through basic anthracene molecule . \\n a series of experimental works dedicated to anthracene molecule suggest that the fermi level in the case of dithiol contacts lies closer to the homo orbital and it is usually found within the homo - lumo gap @xcite . having this on mind \\n , we will take the energy of the homo orbitals as the first reference point , assuming that the fermi level is nearly aligned with the homo level of the planar conformation . \\n as we already mentioned we are focused on rotor - stator molecular systems from a class of anthracene aldehydes . \\n the presence of a flexible side group bound to the central benzene ring in these systems enables fluctuations of the barrier height due to the changes in the position of frontier molecular orbitals ( homo and lumo ) . \\n namely , as the rotor part ( aldehyde group in this case ) undergoes stochastic and thermally activated torsional oscillations the system changes between basically two conformations , planar and a perpendicular one , having different homo and lumo energies . \\n the dependence of the homo and lumo energies on the torsional angle is analyzed in details in our previous work @xcite . \\n it is evident that fluctuations of the position of homo and lumo orbitals with conformational changes occur . \\n also , the temperature effects on the transition probability elaborated in our previous work suggest that the tunneling of electrons via such molecules and interfaces would be governed with the geometry dependent potential barrier under realistic conditions . \\n additionally with the rectangular barrier , we also introduce some more complex sinusoidal position dependence of the tunneling barrier , assuming that the dependence of the frontier orbitals on the geometry of the molecule would result in position dependent tunneling barrier . \\n this position dependence is explained by the effects of the torsional stochastic oscillation of the rotor part , which is situated in the central region , that is not directly attached to the metal leads and thus not significantly affected by the coupling between the molecule and electrodes . under this \\n circumstances the height of the barrier is derived from _ ab initio _ \\n calculations for a free molecule , that could be also considered as one building block of a longer molecular wire . in case \\n when the metal fermi level is aligned with the homo of the planar conformer , the barrier height would be expressed as @xmath2 , where @xmath3 stands for the lumo energy in each particular conformer . \\n special attention is paid on the conformational dependence of the tunneling process , so all the calculations are carried out at different position of the rotor part defined by the dihedral angle in the interval from @xmath4 by a step of @xmath5 . \\n table  [ tab : hlg ] lists the variations of the potential barrier heights @xmath6 with the rotor orientation . \\n .geometry dependence of the barrier height . \\n the dihedral angle describes the orientation of the side aldehyde group with respect to stator anthracene structure . \\n results for each conformer are obtained at b3lyp / lanl2dz theoretical level , changing the dihedral angle by a step of @xmath5 . [ cols=\"<,<,<,<,<,<,<,<,<,<,<\",options=\"header \" , ]     geometry dependence of the molecular electronic structure was analyzed by running dft calculations at different orientations of the side aldehyde group . \\n the obtained results , printed in table [ tab : hlg ] show that the dependence of the positions of the frontier molecular orbitals and the homo - lumo gaps on the geometry of the studied conformers should be taken in consideration when modeling the tunneling barrier in rotor - stator molecular species . \\n delocalization of the charge carrying orbitals of the anthracene aldehyde dithiol molecule in comparison with the basic anthracene is represented in fig . \\n [ fig : fig.1 ] . \\n it is important to note here that experimental values for the frontier molecular orbitals for a series of organic molecular semiconductors , including anthracene molecule , obtained by inverse photoelectron spectroscopy ( ipes ) are reported in @xcite . \\n [ fig : fig.2 ] and  [ fig : fig.3 ] compare the tunneling currents for square and sine potential barrier , respectively , at different orientations of the side groups . \\n changes of the dihedral angles from @xmath7 to @xmath8 lead to variations of the lumo energies which affects the potential barrier heights . \\n the main plot shows the @xmath1 curves at low voltages , ranging from @xmath9 to @xmath10 , while the inset of the plot also includes higher voltages in the range from @xmath11 to @xmath12 . \\n the effects of the side group orientation on the tunneling current are evident and as expected the linear planar conformer has highest conductivity . \\n comparison between the models using square potential barrier and sine barrier shows that when one uses a sine position dependence with strong electrode - molecule coupling , which is usually achieved when dithiol covalent bonds are used , higher tunneling current is observed . while if we consider a completely insulating molecular monolayer , taking the whole length of the molecule to model the length of the potential barrier , the obtained current is by several orders of magnitude lower than the one obtained for sine barrier . \\n however , one should keep on mind that in realistic conditions when the molecule is attached to the leads , the length of the tunneling barrier has somewhat reduced efficient value due to the image force . \\n calculations of the tunneling via lumo orbital with the barrier height equal to one half of the homo - lumo gap , which is satisfied when the fermi level lies in the middle of the molecular energy gap are by several orders of magnitude higher than the ones obtained with the barrier height of the order of the homo - lumo gap . \\n it is important to emphasize that the structural dependence of the tunneling current is evident in all the adopted approaches _ i.e. _ the fluctuations of the position of the charge carrying orbitals caused by rotation of the side aldehyde group decrease the conductance of the planar conformer by several orders of magnitude with respect to the perpendicular one . \\n the distinguishability between the conductance of the planar and the perpendicular conformer was also confirmed by our previous work where coherent transport regime by applying negf formalism was studied @xcite . \\n analysis of the tunneling current in the present work , carried out with several approaches using the values of the potential barrier height obtained by accurate _ \\n ab initio _ \\n calculations accomplishes our previous work confirming that such rotor - stator molecular systems could be implemented as field - controllable single - molecule switches . under realistic conditions when the torsional oscillations are strongly thermally activated and current fluctuations \\n would be observed in this single - molecule device . \\n to avoid such fluctuations , as it was shown in our previous work external electric field could be used to stabilize even the metastable perpendicular state .    in order to test the relevancy of the proposed potential barrier and to inspect transition between direct tunneling to field emission \\n , we adopt the approach from the recent work by beebe et al . \\n @xcite and we plot @xmath13 vs @xmath14 . \\n the inflection points of these curves is used to determine the value of the voltage at which the transition from direct tunneling to field emission occurs . if one compares the values that can be read directly form the plot in fig . \\n [ fig : fig.4 ] for several models of the tunneling barrier , considered in the present work with the values obtained for the basic anthracene by beebe et al . with the transition voltage spectroscopy ( tvs ) \\n higher transition voltage in anthracene with side group would be found . \\n the tvs measurements lead to the value of @xmath15 for the transition voltage value in the afore cited work , while the value obtained for our rotor - stator as can be seen from fig . \\n [ fig : fig.5 ] system is around @xmath10 for the planar conformation . as expected the inflection point \\n is shifted towards lower voltages in the model with lower barrier height . \\n also , the conformational dependence affects the transition voltage which could be concluded from the shift of the curve for perpendicular conformer towards higher voltages with respect to the planar one . \\n the transition voltage obtained here would be probably overestimated since the approximation of the barrier height with the total value of the homo - lumo gap for a free molecule is certainly higher than the actual homo - lumo gap of the molecule bound to electrodes . referring to the electric field effects on the homo - lumo gap , obtained in our previous work \\n one could claim that the biasing field applied along the major molecular axis , parallel to the plane of anthracene fragment would decrease the homo - lumo gap ( see fig . 7 in @xcite ) . \\n this means that the barrier height is expected to be lower than the one consider in our model and thus , the field emission in these metal - molecule - metal junction should be possible at realistically low voltages . \\n in the present paper bridge assisted electron transfer via rotor - stator molecules or molecular interfaces is considered . \\n particularly , tunneling processes through anthracene aldehyde species are investigated . \\n bistability and conformation dependent electron transfer make these species interesting for molecular electronics . \\n wkb approach and simmons formula are applied to calculate the transmission probability and tunneling current , proposing model barriers derived from _ ab initio _ electronic structure calculations . \\n special attention is paid on the dependence of the tunneling current on the molecular geometry . for this purpose a series of electronic structure calculations are carried out at various orientations of the side aldehyde group . to evaluate the tunneling current we consider basically two different model barriers , a rectangular and a sinusoidal barrier . \\n the barrier heights are determined from first principles considering the variations of the homo - lumo gap with the torsional rotation of the rotor part . by considering a sinusoidal barrier \\n we also incorporate the position dependence of the tunneling barrier that is due to the molecular internal structure together with the usual voltage drop arising from the external bias . \\n our results suggest that tunneling processes in this species are strongly dependent on the molecular conformation and the molecular internal structure must be taken into account to derive a realistic model for describing such processes . \\n the fluctuations of the charge carrying orbitals , due to torsional stochastic oscillations of the rotor part of the molecule significantly affect the tunneling current . \\n accounting for the effects of nuclear motion is required by the fact that structural stability of such systems is crucial for prospective practical applications . \\n the present study accompanies our previous work where the coherent transport by application of negf formalism is investigated . within both transport regimes , coherent via strongly coupled delocalized orbital or tunneling via an insulating bridge , a clear difference between the planar and perpendicular molecular conformation is recorded . \\n this confirms that the presence of a side aldehyde group that turns the simple anthracene to a rotor - stator system enriches the interesting and promising properties of the anthracene based molecules , widening the possible areas of application . \\n m. a. reed et al . , science 278 , 252 ( 1997 ) . \\n z. j. donhauser , b. a. mantooth , k. f. kelly , l. a. bumm , j. d. monnell , j. j. stapleton , d. w. price jr . , a. m. rawlett , d. l. allara , j. m. tour , and p. s. weiss , science , 292 , 2303 ( 2001 ) . \\n a. troisi and m. a. ratner , j. am . \\n 124 , 14528 ( 2002 ) . \\n p. e. kornilovitch , a. m. bratkovsky and r. s. williams , phys . rev . \\n b 66 , 245413 ( 2002 ) . a. troisi and m. a. ratner , nanolett . 4 , 591 ( 2004 ) . \\n g. cuniberti , g. fagas , and k. richter , introducing molecular electronics : a brief overview . \\n springer berlin heidelberg , ( 2005 ) . \\n m. ratner , nature nanotech . \\n 8 , 378 ( 2013 ) . \\n l. venkataraman , j. e. klare , c. nuckolls , m. s. hybertsen , and m. l. steigerwald , nature 442 , 904 ( 2006 ) . \\n b. capozzi , q. chen , p. darancet, m. kotiuga, m. buzzeo, j. b. neaton, c. nuckolls , and l. venkataraman , nano lett . \\n 14 , 1400 , ( 2014 ) . \\n a. mitra , i. aleiner , and a. j. millis , phys . \\n b 69 , 245302 ( 2004 ) . \\n j. m. seminario , p. a. derosa and j. l. bastos , j. am . \\n chem . soc . \\n 124 , 10266 ( 2002 ) . \\n p. a. derosa , s. guda and j. m. seminario , j. am . \\n 125 , 14240 ( 2003 ) . \\n j. m. seminario , a. g. zacarias and j. m. tour , j. am . \\n 122 , 3015 ( 2000 ) . \\n j. m. seminario and p. a. derosa , j. am . \\n 123 , 12418 ( 2001 ) . \\n s. k. maiti , phys . \\n e 40 ( 8) , 2730 - 2735 , ( 2008 ) . \\n s. k. maiti , phys . \\n e 61 , 125 , ( 2014 ) . \\n t. yelin , r. vardimon , n. kuritz , r. korytr , a. bagrets , f. evers , l. kronik , and o. tal , nano lett . 13 , 1956 ( 2013 ) . \\n s. j. van der molen and p. liljeroth , j. phys . : \\n matter 22 , 133001 ( 2010 ) . \\n q. fan , ke . \\n q. chen , phys . \\n e 42 , issue 5 , 1492 ( 2010 ) . c. liu , s. kaneko , y. komoto , s. fujii , and m. kiguchi , appl . \\n express 7 , 105201 ( 2014 ) . c. liu , s. kaneko , y. komoto , s. fujii , m. kiguchi , appl . \\n 106 , 103103 ( 2015 ) . \\n moresco , f. et al . \\n 86 , 672 - 675 ( 2001 ) . \\n i. petreska , lj . \\n pejov , lj . \\n kocarev , j. chem . \\n 134 , 014708 ( 2011 ) . \\n a. nitzan , annu . \\n 52 , 681 ( 2001 ) . \\n k. c. liao , l.y . \\n hsu , carleen m. bowers , h. rabitz , and g. m. whitesides , j. am . \\n soc . , 137 , 5948 ( 2015 ) . \\n m. kondratenko , s. r. stoyanov , s. gusarov , a. kovalenko , and r. l. mccreery , j. phys . \\n c 119 , 11286 ( 2015 ) . \\n w. chen , h. li , j. r. widawsky , c. appayee , l. venkataraman , and r. breslow , j. am . \\n 136 , 918 ( 2014 ) . \\n j. g. simmons , j. app . phys . \\n 34 , 6 ( 1963 ) . \\n j. m. beebe , bongsoo kim , j. w. gadzuk , c. d. frisbie and j. g. kushmerick , phys . \\n 97 , 026801 ( 2006 ) j. m. beebe , bongsoo kim , c. d. frisbie and j. g. kushmerick , am . \\n 2 , no . 5 , 827832 ( 2008 ) . \\n d. xiang , y. zhang , f. pyatkov , a. offenhusser and d. mayer , chem . \\n 47 , 4760 , ( 2011 ) . \\n a. d. becke . \\n a 38 , 3098 ( 1988 ) . c. lee , w. yang and r. g. parr , phys \\n b 37 , 785 ( 1988 ) . \\n t. h. dunning jr . and p. j. hay , in modern theoretical chemistry , ed . \\n f. schaefer , iii ( plenum , new york , 1976 ) , vol . 3 , 1 . \\n p. j. hay and w. r. wadt , j. chem . \\n 82 , 270 ( 1985 ) . \\n w. r. wadt and p. j. hay , j. chem . \\n 82 , 284 ( 1985 ) . \\n p. j. hay and w. r. wadt , j. chem . \\n 82 , 299 ( 1985 ) . \\n pejov , m. la rosa and lj . \\n kocarev , chem . \\n 340 , 1 ( 2007 ) . \\n i. petreska , lj . \\n pejov and lj . \\n kocarev , phys . rev . \\n b 78 , 045209 ( 2008 ) . h. \\n b. schlegel , j. comp . chem . 3 , 214 ( 1982 ) . \\n gaussian 03 ( revision b.03 ) , m. j. frisch et al . , \\n gaussian , inc . , pittsburgh pa , ( 2003 ) m. abramowitz and i. a. stegun ( eds . ) . \\n handbook of mathematical functions with formulas , graphs , and mathematical tables , 9th printing . \\n new york : dover , p. 886 \\n p. i. djurovich , e. i. mayo , s. r. forrest , m. e. thompson , organic electronics 10 , 515 ( 2009 ) .',\n",
       "  'abstract': 'tunneling of electrons through rotor - stator anthracene aldehyde molecular interfaces is studied with a combined _ ab initio _ and model approach . \\n molecular electronic structure calculated from first principles is utilized to model different shapes of tunneling barriers . \\n together with a rectangular barrier , we also consider a sinusoidal shape that captures the effects of the molecular internal structure more realistically . \\n quasiclassical approach with the simmons formula for current density is implemented . \\n special attention is paid on conformational dependence of the tunneling current . \\n our results confirm that the presence of the side aldehyde group enhances the interesting electronic properties of the pure anthracene molecule , making it a bistable system with geometry dependent transport properties . \\n we also investigate the transition voltage and we show that confirmation dependent field emission could be observed in these molecular interfaces at realistically low voltages . \\n the present study accompanies our previous work where we investigated the coherent transport via strongly coupled delocalized orbital by application of non - equilibrium green s function formalism .'},\n",
       " {'article': 'ever since the realization of the atom optics quantum kicked rotor ( aoqkr ) @xcite , it has been one of the workhorses for studies of experimental quantum chaos . \\n it has revealed a wide variety of interesting effects including : dynamical localization @xcite , quantum resonances ( qr ) @xcite , quantum accelerator modes @xcite , and quantum ratchets @xcite . \\n the latter are quantum mechanical systems that display directed motion of particles in the absence of unbalanced forces . \\n they are of considerable interest because classical ratchets are the underlying mechanism for some biological motors and nanoscale devices @xcite . \\n recent theoretical @xcite and experimental @xcite studies have demonstrated that a controllable directed current arises in kicked atom systems at qr . \\n a qr occurs when the kicking period is commensurate with the natural periods of the rotor and is characterized by a quadratic growth of the kinetic energy with time . \\n the question of what happens to a ratchet away from resonance was addressed in a recent theoretical paper @xcite . in that work , \\n the authors developed a classical - like ratchet theory and proposed the existence of a one - parameter scaling law that could be used to predict the ratchet current for a wide variety of parameters . \\n it was also shown that an _ inversion _ of the momentum current is possible for some sets of scaling variables .    in this paper , we report the experimental observation of such a ratchet current inversion and the verification of the scaling law for a wide variety of experimental parameters . \\n our experiments were carried out by exposing a bose - einsten condensate ( bec ) to a series of standing wave laser pulses that provided an optical potential periodic in space and time . \\n figure [ rawplot ] shows raw momentum distributions as a function of the pulse period s offset from the first qr and the kick number ( fig . \\n [ rawplot ] ( a ) and ( b ) respectively ) . \\n it can be seen that there are certain values of time offset and kick number where the distribution is weighted more strongly towards negative momentum . \\n this is evidence of a current reversal . \\n furthermore , fig . \\n [ rawplot ] ( a ) and ( b ) contain other similarities . \\n for example , there are parameter regimes where the    s ) ( 10 kicks , @xmath0 , @xmath1 ) , and ( b ) kick number ( @xmath2 , @xmath3 and @xmath1 . ) . \\n each momentum distribution was captured in a separate time - of - flight experiment . \\n note that there are features common to both panels , such as a weighting of the distributions towards positive momenta at small values of the independent variable followed by a tendency towards negative momenta at larger values of this parameter . \\n these features are a manifestation of the fact that the mean momentum or ratchet current can be described by a universal scaling law . \\n , width=9,height=10 ]    momentum distributions tend strongly towards positive momenta , followed by the current reversal regions where the distributions tend negative . \\n this suggests that it may be possible to use a single - parameter theory to understand the behavior of the system . \\n moreover , since the time offset from qr effectively defines a new planck constant @xcite , we can easily switch from the classical to the quantum regime by a simple change of the pulse period @xcite . \\n the dynamics of the aoqkr system can be described by a hamiltonian which in dimensionless units is @xcite : @xmath4 , where @xmath5 is the momentum ( in units of @xmath6 , two photon recoils ) that an atom of mass @xmath7 acquires from short , periodic pulses of a standing wave with a grating vector @xmath8 ( @xmath9 is the spatial period of the standing wave ) . since momentum in this system \\n is only changed in quanta of @xmath6 , we break down @xmath10 as @xmath11 where @xmath12 and @xmath13 are integer and fractional parts of the momentum respectively and @xmath13 , the quasi - momentum , is conserved . \\n other variables are the position @xmath14 ( in units of @xmath15 ) , the continuous time variable @xmath16 ( integer units ) , and the kick number @xmath17 . \\n the pulse period @xmath18 is scaled by @xmath19 ( the half - talbot time ) to give the scaled pulse period @xmath20 . \\n the strength of the kicks is given by @xmath21 , where @xmath22 is the pulse length , @xmath23 is the rabi frequency , and @xmath24 is the detuning of the kicking laser from the atomic transition . to create a ratchet from this hamiltonian \\n it was shown in @xcite that a superposition of two plane waves should be used for the initial state . \\n a successful approach to treating this system close to resonant values of @xmath25 ( i.e. @xmath26 , with @xmath27 integer ) is the so called @xmath28classical theory . here \\n the scaled pulse period is written as @xmath29 , where @xmath30 , and can be shown to play the role of planck s constant . in this case \\n the dynamics can be understood by the classical mapping @xcite , @xmath31 where @xmath32 is the scaled kicking strength , @xmath33 is the scaled momentum variable and @xmath34/2 $ ] is the scaled position exploiting the spatial periodicity of the kick potential . \\n as mentioned above , for the ratchet we start with a superposition of plane waves @xmath35 $ ] , or equivalently a rotor state @xmath36 $ ] . \\n this leads to the position space probability distribution function @xmath37 $ ] . here \\n @xmath38 is an additional phase used to account for the possibility that the initial spatial atomic distribution is shifted in position relative to the applied periodic potential . \\n although the distribution @xmath39 is quantum in origin , in what follows it will be interpreted as a classical probability .     as a function of the scaling variable @xmath40 @xmath17 . in ( a ) \\n @xmath41 was varied by scanning over kick number for different combinations of @xmath42 , @xmath43 and @xmath38 . in panel \\n ( b ) @xmath41 was varied by scanning over @xmath43 with @xmath44 , @xmath45 ( green squares ) , and with @xmath46 , @xmath47 ( red circles ) . also plotted in ( b ) \\n is data from a scan over @xmath42 with @xmath48 , @xmath49 ( blue triangles ) . in both panels , the solid line is the function @xmath50 given by eq . \\n ( [ analytic ] ) . \\n this demonstrates that no matter how @xmath41 is obtained the scaled mean momentum is approximately universal.,width=340,height=359 ]    the original application of @xmath28classical theory to the kicked rotor system showed the existence of a one - parameter scaling law for the mean energy @xcite . \\n this was experimentally verified in the vicinity of the first and second quantum resonances ( @xmath51 and @xmath52 ) in ref . \\n it was found that the scaled energy could be written as @xmath53 where @xmath54 @xmath17 is a scaling variable and @xmath55 and @xmath56 are closed form functions of @xmath41 . \\n recently , the existence of a one - parameter scaling law for the ratchet current using the same scaling parameter @xmath41 was proposed @xcite . \\n one of the notable features of this theory is that it predicts that at some values of the scaling variable ( i.e. certain families of real parameters ) an inversion of momentum current can occur .    in the pendulum approximation @xcite , \\n the motion of the kicked rotor in continuous time is described by the scaled hamiltonian @xmath57 . here \\n @xmath58 is a scaled momentum variable . near the quantum resonance , using the position space probability distribution function @xmath39 , one can calculate @xmath59 . for @xmath60 , eq . \\n ( [ map ] ) gives a phase space dominated by a pendulum - like resonance island of extension @xmath61 @xcite . \\n hence @xmath62 and @xmath63 essentially contribute in the same way giving @xmath64 so that the map in eq . \\n ( [ map ] ) is @xmath65 . with the scaling variable @xmath41 , \\n the average scaled momentum becomes @xmath66 , where    @xmath67    thus the mean momentum ( units of @xmath6 ) expressed in terms of the scaled variables is @xmath68 where @xmath69 can be computed from the above pendulum approximation @xcite . \\n we performed our experiments using a similar set up to that described in @xcite . \\n a bec of about 40000 @xmath70rb atoms was created in the @xmath71 , @xmath72 level using an all - optical trap technique . \\n approximately 5 ms after being released from the trap , the condensate was exposed to a pulsed horizontal standing wave of wavelength @xmath73 . \\n this was formed by two laser beams of wavelength @xmath74 780 nm , detuned @xmath75ghz to the red of the atomic transition . \\n the direction of each beam was aligned at @xmath76 to the vertical to give @xmath77 . with these parameters the primary qr ( half - talbot time @xcite ) occurred at multiples of @xmath78 @xmath79s . \\n each laser beam was passed through an acousto - optic modulator driven by an arbitrary waveform generator . \\n this enabled control of the phase , intensity , and pulse length as well as the relative frequency between the kicking beams . adding two counterpropagating waves differing in frequency by @xmath80 results in a standing wave that moves with a velocity @xmath81 . \\n the initial momentum or quasi - momentum @xmath13 of the bec relative to the standing wave is proportional to @xmath82 , so that by changing @xmath80 the value of @xmath13 could be systematically controlled . \\n the kicking pulse length was fixed at 1.54 @xmath83s , so we varied the intensity rather than the pulse length to change the kicking strength @xmath42 . \\n this was done by adjusting the amplitudes of the rf waveforms driving the kicking pulses , ensuring that the experiments were performed in the raman - nath regime ( the distance an atom travels during the pulse is much smaller than the period of the potential ) . \\n the initial state for the experiment was prepared as a superposition of two momentum states @xmath84 and @xmath85 by applying a long ( @xmath86s ) and very weak standing wave pulse ( bragg pulse ) . by using a pulse of suitable strength , \\n an equal superposition of the two aforementioned atomic states was created ( @xmath87 pulse ) . \\n the bragg pulse was immediately followed by the kicking pulses in which a relative phase of @xmath38 between the beams was applied . \\n this phase was experimentally controlled by adjusting the phase difference between the rf waveforms driving the two aoms . \\n finally the kicked atoms were absorption imaged after @xmath88 ms using a time - of - flight measurement technique to yield momentum distributions like those seen in fig . \\n [ rawplot ] . \\n we now discuss the experiments that were carried out to observe the ratchet effect away from * @xmath51 * resonance . in this case \\n @xmath89 is needed to fulfill the resonance condition @xcite . \\n the measurements involve the determination of the mean momentum of kicked becs for various combinations of the parameters @xmath17 , @xmath42 , @xmath90 and @xmath38 . \\n the measured momentum was then scaled by @xmath91 and is plotted as a function of the scaling variable @xmath41 in fig . \\n [ scaleplot ] . in fig . \\n [ scaleplot](a ) @xmath41 was changed by varying kick number , @xmath17 , while in fig . \\n [ scaleplot](b ) different @xmath41 were obtained by scanning either @xmath43 ( red circles and green squares ) or @xmath42 ( blue triangles ) . \\n the solid line in both panels is a plot of the function @xmath92 given by eq . \\n ( [ analytic ] ) . \\n it can be seen that no matter how @xmath41 is varied , the experimental results are in good agreement with the theory for many different combinations of parameters . in addition , there is a regime over @xmath41 where an inversion of the ratchet current takes place , with a maximum inversion at @xmath93 . \\n interestingly this reversal of the ratchet takes place without altering any of the centers of symmetry of the system . \\n finally , it should be noted that the theory of ref . \\n @xcite also predicts current inversions at higher values of @xmath41 , although these were not seen in the experiments presumably because of dephasing effects such as vibrations and spontaneous emission . \\n even though the @xmath28classical theory assumes @xmath43 is small , the experimental results show that it remains valid for higher values of @xmath43 as well . \\n in fact the window of valid @xmath43 depends on the kick number @xcite , being rather large for small @xmath94 . \\n this is expected from a heisenberg / fourier argument @xcite . \\n ( red crosses ) , @xmath95 ( blue circles ) , @xmath96 ( green diamonds ) , @xmath97 ( black stars ) and @xmath98 ( purple squares ) . \\n the blue solid line is the plot of @xmath99 for @xmath100 and @xmath101 . \\n the dashed lines are the plot of eq . \\n ( [ analytic ] ) with corresponding @xmath43 and the red solid line is the plot of eq.(2 ) in ref . \\n @xcite for @xmath102 and @xmath103 . \\n , width=8,height=7 ]    we also investigated the sensitivity of the finite spread in initial quasi - momentum , @xmath104 to the momentum transfer . \\n figure [ momepsilon ] shows the plot of momentum current as a function of kick number for different values of @xmath43 . \\n the solid blue line is the plot of @xmath99 . \\n the dashed lines are plots of eq . \\n ( [ analytic ] ) for the corresponding experimental parameters . \\n the experimental results show that the farther one goes from resonance the sooner the momentum current turns towards negative values ( current reversal ) . \\n these results are in good agreement with the theory except very close to resonance , where the red dashed curve fits poorly to the red crosses . for this data \\n , we note that the suppression in momentum current is likely to be caused mainly by the effect of the initial spread of quasi - momentum . \\n this phenomenon was also seen in ref . \\n @xcite where the ratchet current for finite @xmath105 was shown to be @xmath106\\\\exp[-2(\\\\pi l \\\\delta\\\\beta s)^2]$ ] . \\n this equation with @xmath107 ( independently estimated from time - of - flight measurements ) is also plotted in fig . \\n [ momepsilon ] ( red solid line ) . \\n it can be seen to agree well with experiment . \\n thus for @xmath108 ( corresponding to an offset from resonance of 0.3 @xmath83s ) , @xmath104 plays an unimportant role in the dynamics of the ratchet . \\n this is because at resonance the total phase the momentum states acquire must be an integer multiple of @xmath109 . \\n any deviation from this condition significantly suppresses the momentum current at longer times . \\n however the momentum state phases away from resonance are already pseudo - random , so the phase changes caused by @xmath104 have a negligible effect . \\n we have performed experiments to observe an off - resonant atomic ratchet by exposing an initial atomic state which was a superposition of two momentum states to a series of standing wave pulses . \\n we measured the mean momentum current as a function of a scaling variable @xmath41 , which contained important pulse parameters such as the offset of the kicking period from resonance , the kick number , and the kick strength . \\n we showed that a scaled version of the mean momentum could be described solely by @xmath41 , a result postulated by a theory based on a classical treatment of the system @xcite . \\n the experiment verified that for certain ranges of @xmath41 the momentum current exhibited an inversion . \\n we also studied the effect of initial quasi - momentum width on the ratchet current away from resonance . \\n this width has a large impact extremely close to resonance , but plays an unimportant role as we go only a little farther from resonance . \\n ultimately one can now control the strength and direction of the ratchet without changing the underlying relative symmetry between the initial state and the potential . \\n this has practical advantages , since it is very easy to control the kicking strength , period , or kick number and hence influence the scaling parameter @xmath41 . \\n another interesting possibility is the investigation of the performance of @xmath28classical ratchet theory as @xmath43 becomes larger . \\n this should allow the crossover from classical to quantum ratchet dynamics @xcite to be better understood . \\n this work was partially supported by the nsf under grant no . \\n sw is very grateful to mark sadgrove for fruitful collaborations , for the cordial hospitality at osu , and for support from the dfg through for760 ( wi 3426/3 - 1 ) , the hgsfp ( gsc 129/1 ) , the cqd and the enable fund of heidelberg university . \\n we also thank to i. talukdar for helpful discussions . \\n 99 f. l. moore , j. c. robinson , c. f. bharucha , b. sundaram , and m. g. raizen , phys . \\n lett . * 75 * , 4598 ( 1995 ) . \\n f. l. moore , j. c. robinson , c. bharucha , p. e. williams , and m. g. raizen , phys . \\n * 73 * , 2974 ( 1994 ) . c. ryu , m. f. anderson , a. vaziri , m. b. d@xmath110arcy , j. m. grossman , k. helmerson , and w. d. phillips , phys . \\n lett . * 96 * , 160403 ( 2006 ) . \\n f. m. izrailev , phys . rep . * 196 * , 299 ( 1990 ) . \\n s. fishman , i. guarneri and l. rebuzzini , phys . \\n lett . * 89 * , 084101 ( 2002 ) ; j. stat . \\n * 110 * , 911 ( 2003 ) . \\n g. behinaein , v. ramareddy , p. ahmadi , and g. s. summy , phys . \\n lett . * 97 * , 244101 ( 2006 ) ; v. ramareddy , g. behinaein , i. talukdar , p. ahmadi and g. s. summy , eur . lett . * 89 * , 33001 ( 2010 ) ; m. k. oberthaler , r. m. godun , m. b. darcy , g. s. summy , and k. burnett , phys . rev . lett . * 83 * , 4447 ( 1999 ) . \\n t. s. monteiro , p. a. dando , n. hutchings , m. isherwood , phys . \\n * 89 * , 194102 ( 2002 ) . i. dana , v. ramareddy , i. talkukdar , and g. s. summy , , phys . \\n lett . * 100 * , 024103 ( 2008 ) . \\n m. sadgrove , m. horikoshi , t. sekimura and k. nakagawa , eur . \\n j. d * 45 * , 229 ( 2007 ) . \\n p. reimann , phys . \\n rep . * 361 * , 57 ( 2002 ) ; r. d. astumian and p. hnggi , phys . today * 55 * , no.11 , 33 ( 2002 ) \\n . m. sadgrove , m. horikoshi , t. sekimura , and k. nakagawa , phys . \\n * 99 * , 043002 ( 2007 ) . \\n t. salger , s. kling , t. hecking , c. geckeler , l. m .- molina , m. weitz , science , * 326 * , 1241 ( 2009 ) .    i. dana and v. roitberg , phys . \\n e. * 76 * , 015201(r ) ( 2007 ) . \\n e. lundh and m. wallin , phys . \\n lett . * 94 * , 110603 ( 2005 ) . \\n a. wickenbrock , d. cubero , n. a. abdul wahab , p. phoonthong , f. renzoni , phys . \\n e * 84 * , 021127 ( 2011 ) . \\n m. sadgrove and s. wimberger , new j. phys . \\n * 11 * , 083027 ( 2009 ) . \\n s. wimberger , i. guarneri and s. fishman , nonlinearity * 16 * , 1381 ( 2003 ) . at qr \\n there is effectively no evolution between the kicks , making the system formally equivalent to the situation where the pulse period and therefore the scaled planck s constant are zero . \\n i. talukdar , r. shrestha and g. s. summy , phys . \\n * 105 * , 054103 ( 2010 ) . m. sadgrove s. wimberger , s. parkins , and r. leonhardt , phys . \\n * 94 * , 174103 ( 2005 ) \\n . s. wimberger , m. sadgrove , s. parkins , and r. leonhardt , phys . rev . a * 71 * , 053404 ( 2005 ) . \\n g. casati and i. guarneri , commun . \\n phys . * 95 * , 121 ( 1984 ) . \\n m. lepers , v. zehnl and j. c. garreau , phys . rev . a * 77 \\n * , 043628 ( 2008 ) . \\n l. deng , e. w. hagley , j. denschlag , j. e. simsarian , mark edwards , charles w. clark , k. helmerson , s. l. rolston , and w. d. phillips , , phys . \\n lett . * 83 * , 5407 ( 1999 ) . m. sadgrove and s. wimberger , adv . at . \\n phys . * 60 * , 315 ( 2011 ) . \\n h. schanz , m .- f . \\n otto , r. ketzmerick , and t. dittrich , phys . \\n lett . * 87 * , 070601 ( 2001 ) .',\n",
       "  'abstract': 'we experimentally investigate the phenomenon of a quantum ratchet created by exposing a bose - einstein condensate to short pulses of a potential which is periodic in both space and time . \\n such a ratchet is manifested by a directed current of particles , even though there is an absence of a net bias force . \\n we confirm a recent theoretical prediction [ m. sadgrove and s. wimberger , new j. phys . * \\n 11 * , 083027 ( 2009 ) ] that the current direction can be controlled by experimental parameters which leave the underlying symmetries of the system unchanged . \\n we demonstrate that this behavior can be understood using a single variable containing many of the experimental parameters and thus the ratchet current is describable using a single universal scaling law .'}]"
      ]
     },
     "execution_count": 9,
     "metadata": {},
     "output_type": "execute_result"
    }
   ],
   "source": [
    "samples = reservoir.get_samples()\n",
    "samples"
   ]
  },
  {
   "cell_type": "code",
   "execution_count": 10,
   "metadata": {},
   "outputs": [],
   "source": [
    "from skopt.space import Integer\n",
    "\n",
    "# Definir o espaço de busca\n",
    "space  = [\n",
    "\tInteger(0, 151642,   name='token0'),\n",
    "\tInteger(0, 151642,   name='token1'),\n",
    "\tInteger(0, 151642,   name='token2'),\n",
    "\tInteger(0, 151642,   name='token3'),\n",
    "\tInteger(0, 151642,   name='token4'),\n",
    "\tInteger(0, 151642,   name='token5'),\n",
    "\tInteger(0, 151642,   name='token6'),\n",
    "\tInteger(0, 151642,   name='token7'),\n",
    "\tInteger(0, 151642,   name='token8'),\n",
    "\tInteger(0, 151642,   name='token9'),\n",
    "\tInteger(0, 151642,   name='token10'),\n",
    "\tInteger(0, 151642,   name='token11'),\n",
    "\tInteger(0, 151642,   name='token12'),\n",
    "\tInteger(0, 151642,   name='token13'),\n",
    "\tInteger(0, 151642,   name='token14'),\n",
    "\tInteger(0, 151642,   name='token15'),\n",
    "\tInteger(0, 151642,   name='token16'),\n",
    "\tInteger(0, 151642,   name='token17'),\n",
    "\tInteger(0, 151642,   name='token18'),\n",
    "\tInteger(0, 151642,   name='token19'),\n",
    "  \tInteger(1, 2000,\t name='temp'), # Define o espaço inteiro para o intervalo [0, 2] com 3 casas decimais\n",
    "\tInteger(1, 1000, \t name='top_k'), # Define o espaço inteiro para o intervalo [0, 1] com 3 casas decimais\n",
    "\tInteger(1, 1000,\t name='top_p') # Define o espaço inteiro para o intervalo [0, 1] com 3 casas decimais\n",
    "]"
   ]
  },
  {
   "cell_type": "code",
   "execution_count": 11,
   "metadata": {},
   "outputs": [],
   "source": [
    "from tqdm import tqdm\n",
    "from skopt.utils import use_named_args\n",
    "import numpy as np\n",
    "\n",
    "@use_named_args(space)\n",
    "def objective(\n",
    "\ttoken0,token1,token2,token3,token4,token5,token6,token7,token8,token9,\n",
    "\ttoken10,token11,token12,token13,token14,token15,token16,token17,token18,token19,\n",
    "\ttemp, top_k, top_p):\n",
    "\t\n",
    "\ttemp = round(temp/1000,3)\n",
    "\ttop_k = round(top_k/1000,3)\n",
    "\ttop_p = round(top_p/1000,3)\n",
    "\t\n",
    "\tbleus = []\n",
    "\tsamples = reservoir.get_samples()\n",
    " \n",
    "\tfor i, ex in tqdm(enumerate(samples), total=len(samples)): \n",
    "\t\ttexto_gerado = create_completion(\n",
    "\t\t\tword_tokenize.decode([token0,token1,token2,token3,token4,token5,token6,token7,token8,token9])+\"\\n\"+\n",
    "\t\t\tex['article']+\n",
    "\t\t\tword_tokenize.decode([token10,token11,token12,token13,token14,token15,token16,token17,token18,token19]),\n",
    "   \t\t\tlen(word_tokenize(ex['abstract']).input_ids),\n",
    "\t\t\ttemp,\n",
    "\t\t\ttop_p,\n",
    "\t\t\ttop_k\n",
    "\t\t)\n",
    "\n",
    "\t\tbleu_score = calcular_bleu(\n",
    "\t\t\ttexto_gerado, \n",
    "\t\t\tex['abstract']\n",
    "\t\t)\n",
    "\t\tbleus.append(bleu_score)\n",
    "\n",
    "\t# BLEU médio\n",
    "\tbleu_medio = np.mean(bleus)\n",
    "\treturn -bleu_medio  # Minimizar => maximizar BLEU"
   ]
  },
  {
   "cell_type": "code",
   "execution_count": 12,
   "metadata": {},
   "outputs": [
    {
     "name": "stderr",
     "output_type": "stream",
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     ]
    }
   ],
   "source": [
    "from skopt import gp_minimize\n",
    "\n",
    "result = gp_minimize(\n",
    "\tfunc=objective,\n",
    "\tdimensions=space,\n",
    "\tn_calls=200,\n",
    "\trandom_state=0,\n",
    "\tn_initial_points=5\n",
    ")"
   ]
  },
  {
   "cell_type": "code",
   "execution_count": 13,
   "metadata": {},
   "outputs": [],
   "source": [
    "token0,token1,token2,token3,token4,token5,token6,token7,token8,token9,token10,token11,token12,token13,token14,token15,token16,token17,token18,token19, melhor_temp, melhor_top_k, melhor_top_p = result.x\n",
    "melhor_bleu = -result.fun\n",
    "\n",
    "melhor_temp = round(melhor_temp/1000,3)\n",
    "melhor_top_k = round(melhor_top_k/1000,3)\n",
    "melhor_top_p = round(melhor_top_p/1000,3)"
   ]
  },
  {
   "cell_type": "code",
   "execution_count": 14,
   "metadata": {},
   "outputs": [
    {
     "name": "stdout",
     "output_type": "stream",
     "text": [
      "===== RESULTADO =====\n",
      "Pre input: \twhile鳜.visit芃’s马上就⽗ offices Footer Horton\n",
      "Pos input: สา.beh铒 lowering spont.Caud 남thèloss\n",
      "Temperatura:  1.037\n",
      "Top_k:        0.35\n",
      "Top_p:        0.552\n",
      "BLEU médio:   0.09593635735476894\n"
     ]
    },
    {
     "data": {
      "image/png": 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",
      "text/plain": [
       "<Figure size 640x480 with 1 Axes>"
      ]
     },
     "metadata": {},
     "output_type": "display_data"
    }
   ],
   "source": [
    "import matplotlib.pyplot as plt\n",
    "from skopt.plots import plot_convergence\n",
    "\n",
    "print(\"===== RESULTADO =====\")\n",
    "print(f\"Pre input: {word_tokenize.decode([token0,token1,token2,token3,token4,token5,token6,token7,token8,token9])}\")\n",
    "print(f\"Pos input: {word_tokenize.decode([token10,token11,token12,token13,token14,token15,token16,token17,token18,token19])}\")\n",
    "print(f\"Temperatura:  {melhor_temp}\")\n",
    "print(f\"Top_k:        {melhor_top_k}\")\n",
    "print(f\"Top_p:        {melhor_top_p}\")\n",
    "print(f\"BLEU médio:   {melhor_bleu}\")\n",
    "\n",
    "plot_convergence(result)\n",
    "plt.show()"
   ]
  },
  {
   "cell_type": "code",
   "execution_count": 15,
   "metadata": {},
   "outputs": [
    {
     "name": "stdout",
     "output_type": "stream",
     "text": [
      " for the lattice at temperature @xmath10 is given by:  ... where it was shown that the lattice spacing and the coupling constant are related via  -the relation between the lattice spacing and the coupling constant is known from the study of the confinement and deconfining transition. \n",
      " the lattice spacing, which was determined using the previous results of the string tension from ref . @xcite to the continuum limit, gives a value for the lattice spacing such that the coupling constant at the temperature 10 is  - the ratio between the lattice spacing and the coupling constant at the temperature 10 is equal to the square root of (the string tension) divided by the \n",
      " 69 . \n",
      "\n",
      " so this was used in the paper @xcite where the continuum limit for the lattice spacing is determined as follows: ... with the critical value of the coupling constant for @xmath29 being @xmath30 @xcite . and the ratio @xmath31 was obtained using data from ref . \n",
      "  to get the value of the lattice spacing, we used results of ref . \n",
      " either directly or via interpolation. \n",
      "\n",
      " the lattice size is determined by the temperature: where the number of sites in the time ( space ) direction is given by 26 per site. so our simulation has a spatial lattice size of 15x15x15x15, which was generated with the tadpole improved symanzik action : parameter @xmath22 is taken here equal to the fourth root of the average p l a u g e p l a u g e . \n",
      " the temperature is given by: where the lattice spacing is determined using results from ref . \n",
      "\n",
      " so this was used in the paper @xcite either directly or via interpolation.  finally, we study the thermal monopole properties in our model by considering the configurations of the lattice gauge field ensembles with various parameters, including the number of sites in the time ( space ) direction, and the temperature.\n",
      "\n",
      " from our earlier studies [tab : lattice_size ] we provide information about the gauge field ensembles and parameters used in our study. \n",
      " from our previous results [tab : lattice_size ] we can see that the lattice size is determined by the temperature: where the number of sites in the time ( space ) direction is given by 26 per site. so our simulation has a spatial lattice size of 15x15x15x15, which was generated with the tadpole improved symanzik action : parameter @xmath22 is taken here equal to the fourth root of the average p l a u g e p l a u g e . \n",
      " the temperature is given by: where the lattice spacing is determined using results from ref . \n",
      "\n",
      " so this was used in the paper @xcite either directly or via interpolation.  finally, we study the thermal monopole properties in our model by considering the configurations of the lattice gauge field ensembles with various parameters, including the number of sites in the time ( space ) direction, and the temperature.\n",
      "\n",
      " from our previous results [tab : lattice_size ] we can see that the lattice size is determined by the temperature: where the number of sites in the time ( space ) direction is given by 26 per site. so our simulation has a spatial lattice size of 15x15x15x15, which was generated with the tadpole improved symanzik action : parameter @xmath22 is taken here equal to the fourth root of the average p l a u g e p l a u g e . \n",
      " the temperature is given by: where the lattice spacing is determined using results from ref . \n",
      "\n",
      " so this was used in the paper @xcite either directly or via interpolation.  finally, we study the thermal monopole properties in our model by considering the configurations of the lattice gauge field ensembles with various parameters, including the number of sites in the time ( space ) direction, and the temperature.\n",
      "\n",
      " from our previous results [tab : lattice_size ] we can see that the lattice size is determined by the temperature: where the number of sites in the time ( space ) direction is given by 26 per site. so our simulation has a spatial lattice size of 15x15x15x15, which was generated with the tadpole improved symanzik action : parameter @xmath22 is taken here equal to the fourth root of the average p l a u g e p l a u g e . \n",
      " the temperature is given by: where the lattice spacing is determined using results from ref . \n",
      "\n",
      " so this was used in the paper @xcite either directly or via interpolation.  finally, we study the thermal monopole properties in our model by considering the configurations of the lattice gauge field ensembles with various parameters, including the number of sites in the time ( space ) direction, and the temperature.\n",
      "\n",
      " from our previous results [tab : lattice_size ] we can see that the lattice size is determined by the temperature: where the number of sites in the time ( space ) direction is given by 26 per site. so our simulation has a spatial lattice size of 15x15x15x15, which was generated with the tadpole improved symanzik action : parameter @xmath22 is taken here equal to the fourth root of the average p l a u g e p l a u g e . \n",
      " the temperature is given by: where the lattice spacing is determined using results from ref . \n",
      "\n",
      " so this was used in the paper @xcite either directly or via interpolation.  finally, we study the thermal monopole properties in our model by considering the configurations of the lattice gauge field ensembles with various parameters, including the number of sites in the time ( space ) direction, and the temperature.\n",
      "\n",
      " from our previous results [tab : lattice_size ] we can see that the lattice size is determined by the temperature: where the number of sites in the time ( space ) direction is given by 26 per site. so our simulation has a spatial lattice size of 15x15x15x15, which was generated with the tadpole improved symanzik action : parameter @xmath22 is taken here equal to the fourth root of the average p l a u g e p l a u g e . \n",
      " the temperature is given by: where the lattice spacing is determined using results from ref . \n",
      "\n",
      " so this was used in the paper @xcite either directly or via interpolation.  finally, we study the thermal monopole properties in our model by considering the configurations of the lattice gauge field ensembles with various parameters, including the number of sites in the time ( space ) direction, and the temperature.\n",
      "\n",
      " from our previous results [tab : lattice_size ] we can see that the lattice size is determined by the temperature: where the number of sites in the time ( space ) direction is given by 26 per site. so our simulation has a spatial lattice size of 15x15x15x15, which was generated with the tadpole improved symanzik action : parameter @xmath22 is taken here equal to the fourth root of the average p l a u g e p l a u g e . \n",
      " the temperature is given by: where the lattice spacing is determined using results from ref . \n",
      "\n",
      " so this was used in the paper @xcite either directly or via interpolation.  finally, we study the thermal monopole properties in our model by considering the configurations of the lattice gauge field ensembles with various parameters, including the number of sites in the time ( space ) direction, and the temperature.\n",
      "\n",
      " from our previous results [tab : lattice_size ] we can see that the lattice size is determined by the temperature: where the number of sites in the time ( space ) direction is given by 26 per site. so our simulation has a spatial lattice size of 15x15x15x15, which was generated with the tadpole improved symanzik action : parameter @xmath22 is taken here equal to the fourth root of the average p l a u g e p l a u g e . \n",
      " the temperature is given by: where the lattice spacing is determined using results from ref . \n",
      "\n",
      " so this was used in the paper @xcite either directly or via interpolation.  finally, we study the thermal monopole properties in our model by considering the configurations of the lattice gauge field ensembles with various parameters, including the number of sites in the time ( space ) direction, and the temperature.\n",
      "\n",
      " from our previous results [tab : lattice_size ] we can see that the lattice size is determined by the temperature: where the number of sites in the time ( space ) direction is given by 26 per site. so our simulation has a spatial lattice size of 15x15x15x15, which was generated with the tadpole improved symanzik action : parameter @xmath22 is taken here equal to the fourth root of the average p l a u g e p l a u g e . \n",
      " the temperature is given by: where the lattice spacing is determined using results from ref . \n",
      "\n",
      " so this was used in the paper @xcite either directly or via interpolation.  finally, we study the thermal monopole properties in our model by considering the configurations of the lattice gauge field ensembles with various parameters, including the number of sites in the time ( space ) direction, and the temperature.\n",
      "\n",
      " from our previous results [tab : lattice_size ] we can see that the lattice size is determined by the temperature: where the number of sites in the time ( space ) direction is given by 26 per site. so our simulation has a spatial lattice size of 15x15x15x15, which was generated with the tadpole improved symanzik action : parameter @xmath22 is taken here equal to the fourth root of the average p l a u g e p l a u g e . \n",
      " the temperature is given by: where the lattice spacing is determined using results from ref . \n",
      "\n",
      " so this was used in the paper @xcite either directly or via interpolation.  finally, we study the thermal monopole properties in our model by considering the configurations of the lattice\n"
     ]
    },
    {
     "data": {
      "text/plain": [
       "0.012173557684781358"
      ]
     },
     "execution_count": 15,
     "metadata": {},
     "output_type": "execute_result"
    }
   ],
   "source": [
    "texto_gerado = create_completion(\n",
    "\t\t\tword_tokenize.decode([token0,token1,token2,token3,token4,token5,token6,token7,token8,token9])+\"\\n\"+\n",
    "\t\t\tsamples[0]['article']+\n",
    "\t\t\tword_tokenize.decode([token10,token11,token12,token13,token14,token15,token16,token17,token18,token19]),\n",
    "   \t\t\tlen(word_tokenize(samples[0]['article']).input_ids),\n",
    "            melhor_temp,\n",
    "            melhor_top_p,\n",
    "            melhor_top_k\n",
    "        )\n",
    "\n",
    "print(texto_gerado)\n",
    "calcular_bleu(\n",
    "\ttexto_gerado, \n",
    "\tsamples[0]['abstract']\n",
    ")"
   ]
  },
  {
   "cell_type": "code",
   "execution_count": 16,
   "metadata": {},
   "outputs": [
    {
     "name": "stdout",
     "output_type": "stream",
     "text": [
      "the properties of the thermal abelian color - magnetic monopoles in the maximally abelian gauge are studied in the deconfinement phase of the lattice @xmath0 gluodynamics . to check universality of the monopole properties we employ the tadpole improved symanzik action . \n",
      " the simulated annealing algorithm combined with multiple gauge copies is applied for fixing the maximally abelian gauge to avoid effects of gribov copies . \n",
      " we compute the density , interaction parameters , thermal mass and chemical potential of the thermal abelian monopoles in the temperature range between @xmath1 and @xmath2 . in comparison with earlier findings our results for these quantities \n",
      " are improved either with respect to effects of gribov copies or with respect to lattice artifacts .\n"
     ]
    }
   ],
   "source": [
    "print(samples[0]['abstract'])"
   ]
  }
 ],
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