Extension of dynamical mean-field theory by inclusion of nonlocal two-site correlations with variable distance
We present a novel approximation scheme for the treatment of strongly correlated electrons in arbitrary crystal lattices. The approach extends the well-known dynamical mean field theory to include nonlocal two-site correlations of arbitrary spatial extent. We extract the nonlocal correlation functions from two-impurity Anderson models where the impurity-impurity distance defines the spatial extent of the correlations included. Translational invariance is fully respected by our approach since correlation functions of any two-impurity cluster are periodically embedded to -space via a Fourier transform. As a first application, we study the two-dimensional Hubbard model on a simple-cubic lattice. We demonstrate how pseudogap formation in the many-body resonance at the Fermi level results from the inclusion of nonlocal correlations. A comparison of the spectral function with the dynamical-cluster approximation shows qualitative agreement of high- as well as low-energy features.
Compounds with strongly correlated electronsColeman (2003); *quintanillaStrongCorr09; Ramakrishnan (2008) are in the focus of modern solid-state research. They usually contain transition metal ions where part of the valence electrons move in narrow bands or are nearly localized. Prominent examples include high-temperature cuprate superconductors,Plakida (2010) frustrated magnetsLacroix et al. (2011) and heavy-fermion systems.Grewe and Steglich (1991); *colemanHeavyFermionMag07
Despite a large effort, various fundamental questions are still open.Norman et al. (2005); Vojta (2009); Grewe and Steglich (1991); *colemanHeavyFermionMag07; Ramakrishnan (2008) The model system of a single transition metal ion immersed into a metallic matrix has essentially been solved by analyticalWiegmann and Tsvelick (1983); *tsvelickExactSIAMII83; *andreiSolutionKondo83; Hewson (1993) and powerful numerical methods.Wilson (1975); *bullaNRGReview08; *hirschQMC86; *wernerContinousTimeQMC06; *whiteDMRG92; Grewe et al. (2008) However, the more general case of regular crystal lattices with strong electron correlations in or near a metallic regime is much more difficult to handle. The large number of relevant electronic states and the interplay of hybridization and interaction effects makes it even difficult to identify relevant degrees of freedom or arrive at low-energy effective models.
An understanding of electronic correlations lies at the heart of most open problems in this field. Although the metallic character of many materials lends hope to the hypothesis that relevant interactions are screened and thus of short range, they can in principle drive correlations over all ranges of spatial distances.
Modern approachesGrewe (1984); *Grewe:lnca83; *grewe:LNCA87; *kuramoto:XNCA85 focused on the dominant role of the local Coulomb repulsion. In particular, dynamical mean-field theoryPruschke et al. (1995); *georges:dmft96; *georgesDMFTreview04; *vollhardtDMFT11 (DMFT) has proven to be very successful. It is capable of describing lattice versions of the Kondo effect in a regime of sizable local magnetic moments and provides valuable insights to the correlation driven Mott-Hubbard metal-to-insulator transition.Pruschke and Peters (2007); *sordiMITPAM07; *held:MottTransPAM_neighHyb00; *pruschkeLowEnergiePAM00; *bulla:MITHM99 These approximations have met with considerable success concerning, for example, one-particle propertiesMatsuura et al. (1998); *kotliarDMFT04; *maiti:165128; *greteKink11; *schmittNFLvHove10; Grewe (2005) or susceptibilities.Zlatic and Horvatic (1990); *jarrellQMCHM92; *jarrell:symmetricPAM95; *kunesTwoDMFT11; *schmittPhD08; *schmittMagnet11
However, many phenomena require the inclusion of nonlocal correlations. Prominent examples are systems near a quantum critical pointStewart (2001); *stewartNFLReview01app06; *siQCHF10; *loehneysenFLQCP07; *sachdevQCP10; *brounQCP08 or cuprate high-temperature superconductors.Plakida (2010) In recent years extensions of DMFT have been put forward to remedy these shortcomings by the inclusion of some spatial correlations between electrons.Maier et al. (2005); *smithSpatialCorrDMFT00; *toschiDGA07; *kataninDGA2dHM09; *rubtsovDualFermion08; *rubtsovDual09; *tremblayTPSC11 In the cluster approaches, the problem is mapped to an effective cluster of few lattice sites and, in analogy to DMFT, this cluster is treated like a complex impurity in a dynamic external field.
These approaches capture short-range correlations quite accurately and have contributed considerably to the understanding of pseudogaps and shadow bands,Huscroft et al. (2001); *moukouriMIT01; *jarrell:QMCMEMNonLocalDMFT01; Vilk (1997); *Scalapino2006; *kyungPseudogap06; *tremblayPseudogap06; Norman et al. (2005); Macridin et al. (2006) as well as to the possible occurrence of quantum critical points.Vidhyadhiraja et al. (2009); *khatamiQCPHM10; *yangQCSC11; Chen et al. (2011)
However, some problems remain in these theories. In cluster DMFTKotliar et al. (2001); *biroli:CDMFTCausality04 (CDMFT), for example, the translational invariance of the crystal lattice is not fully respected. The dynamical cluster approximationHettler et al. (1998); *hettlerDCA00 (DCA) remedies this shortcoming, but the question remains which choice for the size and geometry of the cluster is advantageous.Isidori and Capone (2009) But the most fundamental limitation is the restriction to rather short-ranged correlations.
In this paper we present a novel kind of self-consistent approach to correlated lattice systems which is in principle capable of including nonlocal correlations of arbitrary distance. It extends the well-known DMFT by the inclusion of two-site correlations of all length-scales and is thus termed nonlocal DMFT (NLD). These correlations are incorporated by a mapping of the lattice model onto a multitude of two-impurity Anderson models (TIAM), where the impurity-impurity distance is varied. The translational invariance and crystal symmetries are fully respected by the scheme proposed here.
The details of the mapping between lattice and two-impurity models is presented in Sec. II. As a first application we study in Sec. III the two-dimensional Hubbard model on a square lattice, a model which is usually considered in connection with cuprate superconductors. We utilize the recently developed two-impurity enhanced noncrossing approximationJabben et al. (2011) as the two-impurity solver and analyze the results obtained with respect to the quality of our novel lattice approach and to their physical implications. A short conclusion and outlook is given in Sec. IV.
Ii Self-consistent lattice theory
In order to introduce the ideas underlying our self-consistent scheme we restrict the following discussion to the example of a single-band Hubbard model
We use a mixed representation, where the kinetic energy is expressed in terms of band states with momentum and spin which are created (annihilated) by the operators (). denotes the local single-particle energy and the dispersion is the Fourier transformation of the hopping matrix elements between lattice sites and with lattice vectors and , respectively. The lattice structure, i.e. the type of lattice and topology of the hopping matrix elements, is completely encoded into the dispersion relation . The interaction energy characterized by the Coulomb matrix element is conveniently written in terms of local occupation number operators which measure an electron on site with spin . The lattice constant will serve as the fundamental length scale and the spin index will be dropped whenever possible without ambiguities.
The extension of the novel approach presented here to more general systems with multiple bands and/or more complicated interactions can be readily obtained.
The fundamental quantity of interest is the one-particle Green function which obeys the Dyson equation
which is represented graphically in Fig. 1. The formal solution is given by
The correlated part
incorporates the irreducible self-energy and accounts for the correction to the noninteracting system due to the interaction term proportional to in the Hamiltonian Eq. (1). It describes the interaction-induced, i.e. correlated, part of the propagation process, in which single-particle transfers via elementary hoppings are excluded.
It is useful to re-write the Dyson equation (2) in terms of the lattice -matrix ,
which is commonly defined via
In the last equality the explicit form of Eq. (3) is used.
Processes contributing to the irreducible self-energy can be grouped together according to the nature and degree of correlations they contain. One contribution represents the exact solution of an isolated interacting local site, which is represented by the “atomic” self-energyHubbard (1963) . All other terms incorporate genuine lattice processes. Some of these are captured by the well-known self-energy of the DMFT-approximation, which furnishes a -independent but dynamic contribution . It incorporates loops through the lattice attached at one site at which all local (dynamic) correlations are fully respected. Beyond DMFT, correlations between two or more of these loops are generated by interaction events at different sites and thus constitute nonlocal cumulant corrections.
Organizing these cumulant corrections according to the number of different lattice sites they correlate, the correlation function of Eq. (4) can be expanded as
It is the aim of the present investigation to identify and calculate the self-energy contribution , which contains all nonlocal correlations between any two sites of the lattice. While two-site correlations are thus explicitly included in this scheme, three-site and higher-order nonlocal cumulant corrections with are neglected. The function incorporating these correlations, , will be extracted from solutions of various two-impurity models where the impurity-impurity distance is varied. Then, the Dyson equation (2), respectively its solution Eq. (3), is used to obtain the lattice Green function.
ii.1 Mapping between the lattice and a set of two-impurity models
In order to extract the function which includes two-site correlations, we consider a two-impurity Anderson modelAlexander and Anderson (1964) (TIAM). The two magnetic impurities are immersed with finite distance into a host with a noninteracting conduction band. The Hamiltonian of one such general TIAM with a fixed distance vector is given by
The -operators (-operators) describe local interacting electrons on the impurities at positions (the noninteracting conduction band electrons with momentum ) with spin . The spatial distance between the two impurities is fixed and given by . is the local single-particle energy on each impurity site and are the Coulomb matrix elements of the local () and nonlocal () density-density interactions. The term proportional to is a possible direct single-particle hopping inside the two-impurity cluster and collects additional interactions as, for example, exchange, pair hopping or correlated hopping. The last term represents the hybridization between interacting electrons of the two-site cluster and noninteracting band electrons.
The scheme proposed is capable of properly treating all such terms in the Hamiltonian so that nonlocal Coulomb interaction or long-ranged single-particle hopping matrix elements can in principle be considered. For the present case of the single-band Hubbard model nonlocal Coulomb matrix elements are not included and the single-particle hopping coincides with that of the underlying lattice as specified in the Hamiltonian of Eq. (1).
Since we are only interested in properties of the interacting -electrons neither the hybridization matrix elements nor the dispersion of the band electrons are directly of interest. Only the effective medium for the two-impurity cluster is relevant which is expressed in terms of these parameters as
It represents propagation processes via the noninteracting conduction band in form of irreducible loops starting and ending at the two-site cluster. In our truly self-consistent theory for a lattice model a corresponding effective medium has to be determined by an appropriate mapping between the lattice and the two-impurity model. Therefore, it becomes dressed and takes into account repeated interactions on local shells of other lattice sites.
A Dyson equation for the local two-impurity Green functions is set up as follows
where we used a matrix notation for the spatial components
The correlated part represents the cluster cumulant Green function and takes the interaction matrix elements into account. Therefore, the direct and indirect hopping events via the effective medium are explicitly incorporated in Eq (11).
The Dyson equation (11) can be formally solved to yield
which apart from the matrix structure and the occurrence of the hopping matrix has the same form as in the single-impurity case.Hewson (1993)
It is instructive to formulate the above equations in terms of the full -matrix of the TIAM, thereby establishing an equivalence to the lattice equations (5) to (7). The local Green function can be expressed as
In contrast to the irreducible medium , the -matrix incorporates repeated visits of the two-impurity cluster. The -matrix is thus built up from irreducible loops, accounted for by the inclusion of for steps inside and outside the cluster, and repeated dwellings inside the cluster, where each visit contributes a factor . It can be expressed as
A mapping between the two-impurity and the lattice model is accomplished by connecting the irreducible correlation functions of both approaches. For each nonzero distance vector with solution of the two-impurity model, we identify
|where the matrix elements [cf. Eq. (12)]|
is the Fourier transform of the lattice correlation function of Eq. (4) and the number sites which have a distance to a given site.
The prefactor of in Eq. (16) arises due to the restricted phase-space for scattering in the two-impurity model compared to the lattice situation. In the two-impurity cluster the interaction-induced scattering always transfers the electron from one site to the other at distance . In contrast, in the lattice the scattering process transfers an electron only in a fraction of cases to one specific site with distance .
There is some ambiguity for the correlation function with zero distance . While in the lattice there is only one such function, , there exist many such functions from all the effective two-impurity models, one for each distance . Then the question arises, which of all these functions should be chosen. To this end, we take a constructive approach, where we start from a reference correlation function obtained with the DMFT and add to it all additional correlations of representative two-impurity clusters at different distances
The momentum dependent correlation function of the lattice theory is now given by the inverse Fourier transform
which directly leads to the full lattice Green function via Eq. (3).
As explained after Eq (10), the effective medium in the framework of our self-consistent theory has to be obtained from lattice quantities. This is achieved by identifying the momentum dependent -matrices of both models,
The momentum dependent -matrix incorporates the correct translationally invariant linear combination of two-site propagations with a fixed distance. Inverting the Fourier transform and using Eq. (7) we obtain the -matrix for a two-impurity model with fixed distance
From this the irreducible medium for the two impurity model can be obtained by inverting Eq. (15) and inserting the known expression for .
Lattice and crystal symmetries are completely respected in the present approach. Lattice-translational invariance is incorporated by construction. Even though the two-impurity models are solved for distances in real-space, the correlation functions , which explicitly exclude single-particle hopping, can be periodized for this purpose with the help of a Fourier transform to yield the lattice correlation function . Crystal symmetries are also fully respected since all the two-impurity models for which the distance vectors are generated by point-group transformations, have identical effective media and are therefore identical. Point group symmetries can even be used to decrease the computational cost as only one representative two-impurity model of such a group of symmetry-related points needs to be solved. The solutions of all the others follow by symmetry operations.
We conclude this section by summarizing the steps of the calculation scheme:
Chose a set of representative distance vectors with , one for each set of symmetry-related distance vectors.
Start with an initial guess for the effective media for each distance vector.
Solve different effective two-impurity models, one for each representative distance with the medium . The result are (matrix) Green functions from which the correlation functions are derived via the inversion of Eq. (13),
Go back to step 3 and iterate until convergence is reached.
One-particle spectra of the lattice are then obtained from Eq. (3) in momentum space and the local function via a Fourier transform.
An earlier approach of Schiller and Ingersent also utilizes a two-impurity model to extend the DMFT to include nonlocal correlations.Schiller and Ingersent (1995) However there are various differences to our approach. They consider an expansion in the inverse spatial dimension and consequently employ the two-impurity model only for one specific distance, i.e. nearest-neighbor sites only. Additionally, they identify the irreducible self-energies [cf. Eq. (4)] of the lattice and the two-impurity model. In contrast, we establish the mapping between the lattice and the effective impurity models via the correlation function . This represents a crucial difference, since includes all propagation processes correlated between the two sites via the interaction. Thus, it also incorporates repeated interaction-induced scattering between two sites which are excluded from the irreducible self-energy but need to be accounted for in the lattice Dyson equation (2). An important point concerns the incorporation of the explicit hopping between nearest neighbor sites . In the present approach the single-particle transfers and free propagations through the medium are explicitly separated from correlation effects in both models, cf. Eqs. (2) and (11). This implies for the two-impurity model the hopping to be incorporated into the effective medium [see Eqs. (11) and (15)] and ensures translational invariance. Additionally, any imbalance in the treatment of inter- and intra-cluster hopping in the two-impurity model, as it occurs, for instance, in the CDMFT, is removed.
Iii self-consistent scheme applied to the 2-Hubbard model
In this section we present results for the two-dimensional () Hubbard model (1) obtained with the approximation scheme described in the previous section. We focus on the metallic regime at not too low temperatures. Long-ranged magnetic order and superconducting states are thus excluded, whereas magnetic correlations of finite extent and the precursor regime of a metal-insulator transition are included and accessible.
For the solution of the two-impurity problems we employ a solver based on direct perturbation theory in the hybridizationGrewe et al. (2008); Keiter and Kimball (1970); *grewe:IVperturb81; *keiterMorandiResolventPerturb84 which is an extension of the two-orbital solverGrewe et al. (2009) and which is described elsewhere.Jabben (2010); Jabben et al. (2011) In contrast to the usual noncrossing approximationGrewe (1983b); *Kuramoto:ncaI83; *bickers:nca87a (NCA) this two-impurity enhanced noncrossing approximation includes vertex corrections which allow for the accurate description of finite Coulomb repulsions.
An important requirement for the two-impurity solver is, it needs to be able to treat dynamic non-diagonal effective media .
We study the Hubbard model on a two-dimensional simple-cubic lattice with nearest-neighbor hopping only. The half-bandwidth is used as unit of energy and we set . The noninteracting spectral function of this system is shown in the inset of Fig. 2(a).
In order to investigate the influence of the nonlocal correlations we consider various stages of the scheme differing in the maximum distance to be incorporated into the approximation. This distance is measured with a Manhattan metric indicated by reflecting the minimum number of elementary hoppings between the two sites. For example, the approximation denoted with NLD(1) includes only two-impurity models of nearest-neighbor lattice sites, that is, the set of distance vectors is given by . Accordingly, in NLD(2) this set is augmented with the four next-nearest neighbor distances, i.e. the set of vectors is and so on.
Figure 2 displays the local single-particle spectral function
for three different temperatures and various stages of the approximation. Panel (a) shows the usual DMFT solution, while panels (b) and (c) show the NLD(1) and NLD(2) spectral functions, respectively. The sequence of decreasing temperatures reveals the development of the well known many-body resonance at the Fermi level in DMFT [panel (a)] indicating the formation of low-energy quasiparticles.Grewe (2005)
The inclusion of nonlocal correlations by utilizing NLD(1) leads to the formation of a pseudogap inside this resonance [see panels (b)]. A further inclusion of next-nearest neighbor correlations [panel (c)] the gap widens and the sidepeaks become more pronounced. We cannot definitely decide whether or not a complete gap forms at zero temperature () where the spectral function vanishes at the Fermi energy, as it was found in a recent two-site DCA calculation.Pruschke (2005) Too low temperatures can not be investigated with our impurity solver due to the violation of Fermi liquid properties.Schmitt et al. (2009); Jabben et al. (2011)
Additionally, in the high-energy part of the spectrum the inclusion of additional neighbors seems to bring out more of the van-Hove singularities at of the original unperturbed () spectrum [see inset of Fig. 2(a)].
Inclusion of additional sites with into our NLD-scheme does not produce considerable changes, at least for this choice of parameters. This can be observed in Fig. 3, where spectral functions for a fixed temperature are shown for various maximal distances up to , i.e. including neighbors reachable by up to three transfer processes . The changes become successively smaller and the curves from NLD(2) and NLD(3) are already almost indistinguishable.
Our calculations clearly show the appearance of high sidepeaks at the borders of the pseudogap. The existence of sidepeaks in the low-energy spectrum is in accord with numerical DCA results,Huscroft et al. (2001); *moukouriMIT01; *jarrell:QMCMEMNonLocalDMFT01 where, however, large cluster sizes where necessary to resolve gap and sidepeaks.
We would like to point out, that the sidepeaks in the low-lying quasiparticle regime bear a strong resemblance to what is observed in a related workJabben et al. (2011) for the TIAM. In our opinion we now find a coherent version of the splitting-scenario described there: The direct and the induced effective hopping generate bonding and antibonding molecular-like orbitals amongst different sites. The strength of this strongly depends on the crystal structure since the relevant effective matrix elements vary and oscillate with distance.Jabben et al. (2011) They are also very sensitive to the position of the Fermi level, which sets a scale for such oscillations. The phase-information and coherence of electron propagations which is necessary for such a splitting is fully incorporated into our approach according to Eq. (21).
These aspects also manifest themselves in the sharpening of the high-energy features around when going from NLD(1) to NLD(2,3).
In addition to the bonding-antibonding splitting, an effective antiferromagnetic exchange between neighboring sites is generated which leads to the suppression of Kondo-like correlations. Both effects described above induce a pseudogap and can lead to a splitting of the coherent many-body resonance at the Fermi level. These cases could in principle be distinguished as the splitting due to molecular binding should be linear in , while the magnetic singlet-triplet splitting is proportional to . However, our choice of parameter values implies similar magnitudes for the hopping and the effective exchange , and both effects should be of comparable size here.
An interesting question is, whether the excitations in the vicinity of the Fermi surface form a dispersive band or are narrowly concentrated in -space. We show in Fig. 4 the -resolved spectral function
for along the diagonal -direction in the Brillouin zone. One still recognizes the original cosine-form of a tight-binding band via the positions of the peaks in the projection onto the -plane. However, these peaks develop a considerable width with growing , which indicates that quasiparticle excitations are not well defined away from the Fermi surface. Near the Fermi level two distinct pairs of narrow peaks are visible at wave-vectors . Even though very slight remnants of these peaks are observable at neighboring wave vectors too, their height is rapidly suppressed as moves away from . Since these maxima apparently furnish the spectral weight of the flanks of the pseudogap observable, e.g., in Fig 3, we conclude those side-peaks to be rather localized in -space. Thus, they are a result of increasing lattice coherence at decreasing temperature.
Remarkably, also near the band edges at and with respective energies rather narrow peaks appear on top of the broad resonances connected with the original band. Since they show up only if next-nearest neighbors are included, i.e. in NLD(2) but not in NLD(1) (and DMFT), we attribute them to next-nearest neighbor correlations, possibly of magnetic nature. A participation of an indirect binding effect due to the repeated action of the transfer , i.e. a molecular orbital-like effect, can also not be excluded with our choice of parameters.
Up to now a symmetric situation was investigated, in which a possible Mott-Hubbard gap as well as a possible pseudogap in the low-energy quasiparticle regime both were to open around the Fermi-level. Both effects can be separated and identified individually by moving away from half-filling, i.e. with increasing doping. Equivalently, we increase the Coulomb-repulsion beyond the value and keep all other parameters fixed.
Calculations for such particle-hole asymmetric situations are shown in Fig. 5. Panel (a) displays the formation of a Mott-Hubbard gap at positive energies with increasing as calculated with the DMFT-approximation. As expected, the center of the incipient gap moves away from the Fermi level by an amount proportional to while the many-body resonance remains pinned at the Fermi level.
Figure 5(b) shows results of NLD(1)-calculations for the same values of . The Mott-Hubbard gap forms at positive energies in a similar fashion as in the DMFT-results of panel (a). Additionally, a pseudogap emerges in the many-body resonance at the Fermi level as it was already found in earlier work.Vidhyadhiraja et al. (2009); *khatamiQCPHM10; *yangQCSC11; Chen et al. (2011); Macridin et al. (2006); Lin et al. (2010); *stanescuCDMFTMIT06; *maier:NCAIntersiteCorr00; Huscroft et al. (2001); *moukouriMIT01; *jarrell:QMCMEMNonLocalDMFT01; Vilk (1997); *Scalapino2006; *kyungPseudogap06; *tremblayPseudogap06
The last part (c) of Fig. 5 shows the effect of including more neighbors in our NLD(i)-scheme for fixed Coulomb interaction . One again recognizes the dominant role of nearest-neighbor correlations since the spectra with all differ considerably from the DMFT-result. The low-energy region seems to be converged for , and the inclusion of next-nearest neighbors apparently smoothens the spikes around the pseudogap.
In contrast, the inclusion of next-next-nearest neighbors () still has considerable impact on the high-energy features at negative energies while at positive energies only small differences are induced. This apparently indicates a reduced hybridization and corresponding band narrowing for states in the vicinity of the negative band edge. The importance of lattice structure, coherence and correlations for the possible development of hybridization gaps and band splittings as they were already discussed in the symmetric case is evident from these results.
The longer-ranged correlations also seem to work in favor of restoring particle-hole symmetry in the low-energy region [see inset of Fig. 5(c)], a phenomenon which is also discussed in connection with the cuprate superconductors.Vidhyadhiraja et al. (2009); *khatamiQCPHM10; *yangQCSC11; Chen et al. (2011); Chakraborty et al. (2010)
Figure 6 compares a NLD(3) spectral function for finite doping and with a spectrum obtained from a DCA calculation as it was published in Fig. 5 of Ref. Chen et al., 2011. The qualitative features of both approaches nicely agree: the humps and minima visible in the DCA spectra translate to corresponding but more pronounced features in the NLD(3). Given the different nature of the two approximations, this provides additional evidence for the physical nature of the observed structures.
The magnitude of the pseudogap is of the same order in both approaches, although the DCA result is slightly larger and the low-energy spectrum much more asymmetric. One reason for this can be found in the enhanced two-impurity noncrossing approximation as the two-impurity solver, which is known to produce a too small many-body low-energy scale for the SIAM. This is especially relevant for the low-energy region and also translates to self-consistent approximations (see, e.g. Ref. Grete et al., 2011).
The different temperatures of both calculations should not be relevant for the qualitative features as is already rather low and further decreasing it will only slightly deepen the pseudogap.
However, a qualitative difference between the two calculations is found in the different fillings which in general strongly influences the low-energy spectral function. The analysis in Ref. Chen et al., 2011 revealed that decreasing the filling from to (for otherwise identical parameters) leads to a spectral function which is nearly particle-hole symmetric at low energies and does not exhibit a pseudogap. In this light, the NLD(3) spectral function for with a nearly symmetric low-energy spectrum and a small pseudogap represent a plausible intermediate solution.
We have proposed a novel general and nonperturbative scheme for the treatment of correlated electron systems on crystal lattices. Our approach represents an extension of the well-known DMFT to include nonlocal two-site correlations with arbitrary spatial extent.
The self-consistent formulation establishes a mapping between nonlocal two-site correlations of the lattice model and the equivalent functions of various two-impurity Anderson models with varying distance. The two-impurity models are solved in real-space, but the extracted correlation functions are transformed into momentum space via a Fourier transform. Thereby translational invariance is built into our scheme by construction.
Most important, the spatial range of correlations which are explicitly included in the treatment is unrestricted in principle. It corresponds to the maximum impurity-impurity distance in an effective TIAM which is solved in our approach, and is therefore only limited by the accuracy of the two-impurity solver.
As a first application, we applied our scheme to the Hubbard model on a two-dimensional simple-cubic lattice. We found that the leading nonlocal correlations produce a pseudogap in the low-energy single-particle excitation spectrum as it is to be expected.Vidhyadhiraja et al. (2009); *khatamiQCPHM10; *yangQCSC11; Chen et al. (2011); Macridin et al. (2006); Lin et al. (2010); *stanescuCDMFTMIT06; *maier:NCAIntersiteCorr00; Huscroft et al. (2001); *moukouriMIT01; *jarrell:QMCMEMNonLocalDMFT01; Vilk (1997); *Scalapino2006; *kyungPseudogap06 Moreover, pronounced side-peaks occur as a signature of increasing coherence. In a situation without particle-hole symmetry we could clearly discriminate between the Mott-Hubbard gap induced by mostly local atomic correlations and the pseudogap, which is found in the many-body resonance at the Fermi level. We have also demonstrated that the inclusion of correlations over larger distances brings out more details of the excitation spectra in the high-energy region.
Additionally, our method compares very well to results from the DCA. The spectral functions of both approaches exhibit similar qualitative features for finite doping, although they are more pronounced in our scheme. Also, the pseudogap obtained within both approaches is of the same magnitude.
Thus, the scheme presented opens an excellent perspective for more detailed investigations of systems where nonlocal correlations play an important role. These include phase transitions and critical phenomena in general, and quantum critical points in particular, as they are found, for example, in heavy fermion compounds or cuprate superconductors.
Also, the calculation of nontrivial critical exponents and their scaling behaviorRohringer et al. (2011) seems to be in reach using this new approach. In some cases it will nevertheless be necessary to include higher-order irreducible correlations beyond those between only two sites. This will be of particular importance, when complicated ground states involving correlations on plaquettes of sites or general resonating valence bond-states are under consideration.Yang et al. (2010); *nature08942; *1173.full
Acknowledgements.We thank Eberhard Jakobi for fruitful discussions, Kuang-Shing Chen for providing us with the DCA data shown in Fig. 6, and the NIC, Forschungszentrum Jülich, for their supercomputer support under Project No. HDO00. SS acknowledges financial support from the Deutsche Forschungsgemeinschaft under Grant No. AN 275/6-2.
- Coleman (2003) P. Coleman, Ann. Henri Poincare, Suppl. 2 4, S559 (2003).
- Quintanilla and Hooley (2009) J. Quintanilla and C. Hooley, Physics World 22, 32 (2009).
- Ramakrishnan (2008) T. V. Ramakrishnan, Current Science 95, 1284 (2008).
- Plakida (2010) N. Plakida, High-Temperature Cuprate Superconductors, vol. 166 of Springer Series in solid-state sciences (Springer, 2010).
- Lacroix et al. (2011) C. Lacroix, P. Mendels, and F. Mila, eds., Introduction to Frustrated MagnetismIntroduction to Frustrated Magnetism, vol. 164 of Springer Series in Solid-State Sciences (Springer, 2011).
- Grewe and Steglich (1991) N. Grewe and F. Steglich, Handbook on the Physics and Chemistry of Rare Earths (North-Holland, 1991), vol. 14, p. 343.
- Coleman (2007) P. Coleman, Handbook of Magnetism and Advanced Magnetic Materials (John Wiley and Sons, Ltd., Weinheim, 2007), vol. 1, chap. Heavy Fermions: electrons at the edge of magnetism, pp. 95–148.
- Norman et al. (2005) M. R. Norman, D. Pines, and C. Kallin, Adv. Phys. 54, 715 (2005).
- Vojta (2009) M. Vojta, Nat. Phys. 5, 623 (2009).
- Wiegmann and Tsvelick (1983) P. B. Wiegmann and A. M. Tsvelick, J. Phys. C 16, 2281 (1983).
- Tsvelick and Wiegmann (1983) A. M. Tsvelick and P. B. Wiegmann, J. Phys. C 16, 2321 (1983).
- Andrei et al. (1983) N. Andrei, K. Furuya, and J. H. Lowenstein, Rev. Mod. Phys. 55, 331 (1983).
- Hewson (1993) A. C. Hewson, The Kondo Problem to Heavy Fermions (Cambridge University Press, Cambridge, 1993).
- Wilson (1975) K. G. Wilson, Rev. Mod. Phys. 47, 773 (1975).
- Bulla et al. (2008) R. Bulla, T. Costi, and T. Pruschke, Rev. Mod. Phys. 80, 395 (2008).
- Hirsch and Fye (1986) J. E. Hirsch and R. M. Fye, Phys. Rev. Lett. 56, 2521 (1986).
- Werner et al. (2006) P. Werner, A. Comanac, L. de’ Medici, M. Troyer, and A. J. Millis, Phys. Rev. Lett. 97, 076405 (2006).
- White (1992) S. R. White, Phys. Rev. Lett. 69, 2863 (1992).
- Grewe et al. (2008) N. Grewe, S. Schmitt, T. Jabben, and F. B. Anders, J. Phys.: Condens. Matter 20, 365217 (2008).
- Grewe (1984) N. Grewe, Solid State Commun. 50, 19 (1984).
- Grewe (1983a) N. Grewe, Z. Phys. B 52, 193 (1983a).
- Grewe (1987) N. Grewe, Z. Phys. B 67, 323 (1987).
- Kuramoto (1985) Y. Kuramoto, in Theory of heavy fermions and valence fluctuation, edited by T. Kasuka and T. Saso (Springer, Berlin, 1985), vol. 62 of Springer series in solid state sciences, pp. 152–161.
- Pruschke et al. (1995) T. Pruschke, M. Jarrell, and J. Freericks, Adv. Phys. 44, 187 (1995).
- Georges et al. (1996) A. Georges, G. Kotliar, W. Krauth, and M. J. Rozenberg, Rev. Mod. Phys. 68, 13 (1996).
- A.Georges (2004) A.Georges, in Lectures on the physics of highly correlated electron systems VIII, edited by A.Avella and F.Mancini (2004), vol. 715 of AIP Conf. Proc., pp. 3–74.
- Vollhardt (2011) D. Vollhardt, Ann. Phys. (Berlin) pp. 1–23 (2011).
- Pruschke and Peters (2007) T. Pruschke and R. Peters, J. Magn. Magn. Mater. 310, 935 (2007).
- Sordi et al. (2007) G. Sordi, A. Amaricci, and M. J. Rozenberg, Phys. Rev. Lett. 99, 196403 (2007).
- Held and Bulla (2000) K. Held and R. Bulla, Eur. Phys. J. B 17, 7 (2000).
- Pruschke et al. (2000) T. Pruschke, R. Bulla, and M. Jarrell, Phys. Rev. B 61, 12799 (2000).
- Bulla (1999) R. Bulla, Phys. Rev. Lett. 83, 136 (1999).
- Matsuura et al. (1998) A. Y. Matsuura, H. Watanabe, C. Kim, S. Doniach, Z.-X. Shen, T. Thio, and J. W. Bennett, Phys. Rev. B 58, 3690 (1998).
- Kotliar and Vollhardt (2004) G. Kotliar and D. Vollhardt, Physics Today 57, 53 (2004).
- Maiti et al. (2007) K. Maiti, R. S. Singh, and V. R. R. Medicherla, Phys. Rev. B 76, 165128 (2007).
- Grete et al. (2011) P. Grete, S. Schmitt, C. Raas, F. B. Anders, and G. S. Uhrig, Phys. Rev. B 84, 205104 (2011).
- Schmitt (2010) S. Schmitt, Phys. Rev. B 82, 155126 (2010).
- Grewe (2005) N. Grewe, Ann. Phys. (Leipzig) 14, 611 (2005).
- Zlatic and Horvatic (1990) V. Zlatic and B. Horvatic, Solid State Commun. 75, 263 (1990).
- Jarrell (1992) M. Jarrell, Phys. Rev. Lett. 69, 168 (1992).
- Jarrell (1995) M. Jarrell, Phys. Rev. B 51, 7429 (1995).
- Kuneš (2011) J. Kuneš, Phys. Rev. B 83, 085102 (2011).
- Schmitt (2009) S. Schmitt, Ph.D. thesis, TU Darmstadt (2009), available at http://tuprints.ulb.tu-darmstadt.de/1264/.
- Schmitt et al. (2011) S. Schmitt, N. Grewe, and T. Jabben, Phys. Rev. B 85, 024404 (2012).
- Stewart (2001) G. R. Stewart, Rev. Mod. Phys. 73, 797 (2001).
- Stewart (2006) G. R. Stewart, Rev. Mod. Phys. 78, 743 (2006).
- Si and Steglich (2010) Q. Si and F. Steglich, Science 329, 1161 (2010).
- v. Lohneysen et al. (2007) H. v. Lohneysen, A. Rosch, M. Vojta, and P. Wolfle, Rev. Mod. Phys. 79, 1015 (2007).
- Sachdev (2010) S. Sachdev, Phys. Status Solidi B 247, 537 (2010).
- Broun (2008) D. M. Broun, Nature Physics 4, 170 (2008).
- Maier et al. (2005) T. Maier, M. Jarrell, T. Pruschke, and M. H. Hettler, Rev. Mod. Phys. 77, 1027 (2005).
- Smith and Si (2000) J. L. Smith and Q. Si, Phys. Rev. B 61, 5184 (2000).
- Toschi et al. (2007) A. Toschi, A. A. Katanin, and K. Held, Phys. Rev. B 75, 045118 (2007).
- Katanin et al. (2009) A. A. Katanin, A. Toschi, and K. Held, Phys. Rev. B 80, 075104 (2009).
- Rubtsov et al. (2008) A. N. Rubtsov, M. I. Katsnelson, and A. I. Lichtenstein, Phys. Rev. B 77, 033101 (2008).
- Rubtsov et al. (2009) A. N. Rubtsov, M. I. Katsnelson, A. I. Lichtenstein, and A. Georges, Phys. Rev. B 79, 045133 (2009).
- Tremblay (2012) A.-M. Tremblay, Theoretical methods for Strongly Correlated Systems (Springer Verlag, 2012), chap. Two-Particle-Self-Consistent Approach for the Hubbard Model.
- Huscroft et al. (2001) C. Huscroft, M. Jarrell, T. Maier, and A.-N. Tahvildarzadeh, Phys. Rev. Lett. 86, 139 (2001).
- Moukouri and Jarrell (2001) S. Moukouri and M. Jarrell, Phys. Rev. Lett. 87, 167010 (2001).
- Jarrell et al. (2001) M. Jarrell, T. Maier, C. Huscroft, and S. Moukouri, Phys. Rev. B 64, 195130 (2001).
- Vilk (1997) Y. M. Vilk, Phys. Rev. B 55, 3870 (1997).
- Scalapino (2007) D. J. Scalapino, Handbook of High Temperature Superconductivity (Springer, Berlin, 2007), chap. Numerical Studies of the 2D Hubbard Model, p. 495.
- Kyung et al. (2006) B. Kyung, S. S. Kancharla, D. Sénéchal, A.-M. S. Tremblay, M. Civelli, and G. Kotliar, Phys. Rev. B 73, 165114 (2006).
- Tremblay et al. (2006) A.-M. S. Tremblay, B. Kyung, and D. SÃ©nÃ©chal, Low Temp. Phys. 32, 424 (2006).
- Macridin et al. (2006) A. Macridin, M. Jarrell, T. Maier, P. R. C. Kent, and E. D’Azevedo, Phys. Rev. Lett. 97, 036401 (2006).
- Vidhyadhiraja et al. (2009) N. S. Vidhyadhiraja, A. Macridin, C. Sen, M. Jarrell, and M. Ma, Phys. Rev. Lett. 102, 206407 (2009).
- Khatami et al. (2010) E. Khatami, K. Mikelsons, D. Galanakis, A. Macridin, J. Moreno, R. T. Scalettar, and M. Jarrell, Phys. Rev. B 81, 201101 (2010).
- Yang et al. (2011) S.-X. Yang, H. Fotso, S.-Q. Su, D. Galanakis, E. Khatami, J.-H. She, J. Moreno, J. Zaanen, and M. Jarrell, Phys. Rev. Lett. 106, 047004 (2011).
- Chen et al. (2011) K.-S. Chen, S. Pathak, S.-X. Yang, S.-Q. Su, D. Galanakis, K. Mikelsons, M. Jarrell, and J. Moreno, Phys. Rev. B 84, 245107 (2011).
- Kotliar et al. (2001) G. Kotliar, S. Y. Savrasov, G. Pálsson, and G. Biroli, Phys. Rev. Lett. 87, 186401 (2001).
- Biroli et al. (2004) G. Biroli, O. Parcollet, and G. Kotliar, Phys. Rev. B 69, 205108 2004).
- Hettler et al. (1998) M. H. Hettler, A. N. Tahvildar-Zadeh, M. Jarrell, T. Pruschke, and H. R. Krishnamurthy, Phys. Rev. B 58, R7475 (1998).
- Hettler et al. (2000) M. H. Hettler, M. Mukherjee, M. Jarrell, and H. R. Krishnamurthy, Phys. Rev. B 61, 12739 (2000).
- Isidori and Capone (2009) A. Isidori and M. Capone, Phys. Rev. B 79, 115138 (2009).
- Jabben et al. (2011) T. Jabben, N. Grewe, and S. Schmitt, Phys. Rev. B 85, 045133 (2012).
- Hubbard (1963) J. Hubbard, Proc. Roy. Soc. A 276, 238 (1963).
- Alexander and Anderson (1964) S. Alexander and P. W. Anderson, Phys. Rev. 133, A1594 (1964).
- Schiller and Ingersent (1995) A. Schiller and K. Ingersent, Phys. Rev. Lett. 75, 113 (1995).
- Keiter and Kimball (1970) H. Keiter and J. C. Kimball, Phys. Rev. Lett. 25, 672 (1970).
- Grewe and Keiter (1981) N. Grewe and H. Keiter, Phys. Rev. B 24, 4420 (1981).
- Keiter and Morandi (1984) H. Keiter and G. Morandi, Phys. Rep. 109, 227 (1984).
- Grewe et al. (2009) N. Grewe, T. Jabben, and S. Schmitt, Eur. Phys. J. B 68, 23 (2009).
- Jabben (2010) T. Jabben, Ph.D. thesis, TU Darmstadt (2010).
- Grewe (1983b) N. Grewe, Z. Phys. B 53, 271 (1983b).
- Kuramoto (1983) Y. Kuramoto, Z. Phys. B 53, 37 (1983).
- Bickers (1987) N. E. Bickers, Rev. Mod. Phys. 59, 845 (1987).
- Pruschke (2005) T. Pruschke, Physica B 359-361, 633 (2005).
- Schmitt et al. (2009) S. Schmitt, T. Jabben, and N. Grewe, Phys. Rev. B 80, 235130 (2009).
- Lin et al. (2010) N. Lin, E. Gull, and A. J. Millis, Phys. Rev. B 82, 045104 (2010).
- Stanescu et al. (2006) T. D. Stanescu, M. Civelli, K. Haule, and G. Kotliar, Ann. Phys. 321, 1682 (2006).
- Maier et al. (2000) T. Maier, M. Jarrell, T. Pruschke, and J. Keller, Eur. Phys. J. B 13, 613 (2000).
- Chakraborty et al. (2010) S. Chakraborty, D. Galanakis, and P. Phillips, Phys. Rev. B 82, 214503 (2010).
- Rohringer et al. (2011) G. Rohringer, A. Toschi, A. Katanin, and K. Held, Phys. Rev. Lett. 107, 256402 (2011).
- Yang et al. (2010) H.-Y. Yang, A. M. Läuchli, F. Mila, and K. P. Schmidt, Phys. Rev. Lett. 105, 267204 (2010).
- Meng et al. (2010) Z. Y. Meng, T. C. Lang, S. Wessel, F. F. Assaad, and A. Muramatsu, Nature 464, 847 (2010).
- Yan et al. (2001) S. Yan, D. A. Huse, and S. R. White, Science 332, 1173 (2001).