## Abstract

We analyze the measured optical conductivity spectra using the density-functional-theory-based electronic structure calculation and density-matrix renormalization group calculation of an effective model. We show that, in contrast to a conventional description, the Bose-Einstein condensation of preformed excitons occurs in Ta2NiSe5, despite the fact that a noninteracting band structure is a band-overlap semimetal rather than a small band-gap semiconductor. The system above the transition temperature is therefore not a semimetal but rather a state of preformed excitons with a finite band gap. A novel insulator state caused by the strong electron-hole attraction is thus established in a real material.

Original language | English |
---|---|

Article number | 247602 |

Journal | Physical review letters |

Volume | 120 |

Issue number | 24 |

DOIs | |

Publication status | Published - 2018 Jun 14 |

Externally published | Yes |

## ASJC Scopus subject areas

- Physics and Astronomy(all)

## Access to Document

## Other files and links

## Fingerprint Dive into the research topics of 'Strong Coupling Nature of the Excitonic Insulator State in Ta2NiSe5'. Together they form a unique fingerprint.

## Cite this

- APA
- Standard
- Harvard
- Vancouver
- Author
- BIBTEX
- RIS

*Physical review letters*,

*120*(24), [247602]. https://doi.org/10.1103/PhysRevLett.120.247602

**Strong Coupling Nature of the Excitonic Insulator State in Ta2NiSe5.** / Sugimoto, Koudai; Nishimoto, Satoshi; Kaneko, Tatsuya; Ohta, Yukinori.

Research output: Contribution to journal › Article › peer-review

*Physical review letters*, vol. 120, no. 24, 247602. https://doi.org/10.1103/PhysRevLett.120.247602

**Strong Coupling Nature of the Excitonic Insulator State in Ta2NiSe5**. In: Physical review letters. 2018 ; Vol. 120, No. 24.

}

TY - JOUR

T1 - Strong Coupling Nature of the Excitonic Insulator State in Ta2NiSe5

AU - Sugimoto, Koudai

AU - Nishimoto, Satoshi

AU - Kaneko, Tatsuya

AU - Ohta, Yukinori

N1 - Funding Information: Ta 2 NiSe 5 Sugimoto Koudai 1 Nishimoto Satoshi 2,3 Kaneko Tatsuya 4 Ohta Yukinori 5 Center for Frontier Science, 1 Chiba University , Chiba 263-8522, Japan Department of Physics, 2 Technical University Dresden , 01069 Dresden, Germany 3 Institute for Theoretical Solid State Physics , IFW Dresden, 01171 Dresden, Germany Computational Condensed Matter Physics Laboratory, 4 RIKEN , Wako, Saitama 351-0198, Japan Department of Physics, 5 Chiba University , Chiba 263-8522, Japan 14 June 2018 15 June 2018 120 24 247602 29 April 2018 30 August 2017 © 2018 American Physical Society 2018 American Physical Society We analyze the measured optical conductivity spectra using the density-functional-theory-based electronic structure calculation and density-matrix renormalization group calculation of an effective model. We show that, in contrast to a conventional description, the Bose-Einstein condensation of preformed excitons occurs in Ta 2 NiSe 5 , despite the fact that a noninteracting band structure is a band-overlap semimetal rather than a small band-gap semiconductor. The system above the transition temperature is therefore not a semimetal but rather a state of preformed excitons with a finite band gap. A novel insulator state caused by the strong electron-hole attraction is thus established in a real material. Japan Society for the Promotion of Science 10.13039/501100001691 JP15H06093 JP17K05530 JP18K13509 Deutsche Forschungsgemeinschaft 10.13039/501100001659 SFB 1143 It has been commonly understood [1–4] that excitonic condensation occurs when electrons and holes in a small band-overlap semimetal or a small band-gap semiconductor form pairs (or excitons) owing to the attractive Coulomb interaction and condense into a quantum state with macroscopic phase coherence. The excitonic condensation in semimetallic systems can be described in analogy with the BCS theory of superconductors, and that in semiconducting systems can be discussed in terms of the Bose-Einstein condensation (BEC) of preformed excitons [5–7] . A well-known phase diagram [8] is depicted in Fig. 1 . 1 10.1103/PhysRevLett.120.247602.f1 FIG. 1. Schematic representation of the conventional phase diagram of an excitonic insulator [8] . The band gap E g in the noninteracting band structure is either positive (semiconducting) or negative (semimetallic). The crossover between the semimetallic and semiconducting states at finite temperatures ( T ) is indicated by the dashed line. In this Letter, we will show that this conventional picture established half a century ago [8] is, in fact, seriously violated in a candidate material Ta 2 NiSe 5 recently found [9–13] . Namely, based on the analyses of the measured optical conductivity spectra [13–15] , we will show that the excitonic BEC occurs in Ta 2 NiSe 5 , despite the fact that the noninteracting band structure is a band-overlap semimetal rather than a small band-gap semiconductor. In other words, even though the noninteracting band structure is semimetallic, the system above the transition temperature ( T c ) is not a semimetal but rather a state of preformed excitons with a finite band gap, exhibiting a variety of intriguing physical properties. A novel insulator state caused by the strong electron-hole attraction is thus established, which may be contrasted with a Mott insulator state caused by the strong electron-electron repulsion. Let us first review essential physical properties of Ta 2 NiSe 5 briefly. This material has a layered structure stacked loosely by a weak van der Waals interaction, and, in each layer, Ni single chains and Ta double chains run along the a axis of the lattice to form a quasi-one-dimensional (1D) chain structure [16] . The observed resistivity shows a semiconducting behavior over a wide temperature range up to ∼ 500 K [17] , with a quasi-1D anisotropic electron conduction [13] . An anomaly in the resistivity appears at T c ≃ 328 K , which is associated with a second-order structural phase transition from the orthorhombic to the monoclinic phase [17] . The magnetic susceptibility exhibits diamagnetism in a wide temperature range and shows a sudden drop (being more negative) below T c [17] . The angle-resolved photoemission spectroscopy (ARPES) experiment [9,11] showed that, by lowering the temperature, the flatness of the top of the valence band is enhanced and the size of the band gap becomes wider, thereby suggesting that the excitonic insulator state is realized as the ground state of this material [9] . Kaneko et al. [10] then made the density-functional-theory (DFT) -based electronic structure calculations for the orthorhombic phase of Ta 2 NiSe 5 and found that the system is a direct-gap semiconductor with the gap minimum at the Γ point of the Brillouin zone. No hybridization occurs between the top of the valence band and the bottom of the conduction band, which belong to different irreducible representations at the Γ point. The effective three-chain Hubbard model was then constructed to reproduce three bands near the Fermi level. This model, together with the phonon degrees of freedom [18] , was analyzed by the mean-field approximation, and the ground-state and finite-temperature phase diagrams were obtained to show that the BEC of excitons cooperatively induces the structural phase transition [10] . The spontaneous hybridization between the conduction and valence bands well reproduces the flattening of the top of the valence band observed in the ARPES experiment [10] . A number of physical quantities have also been discussed along this line [19–22] . Recently, a comparative experimental study of the optical conductivity spectra of Ta 2 NiSe 5 and Ta 2 NiS 5 was made [14,15] , which provided us with an unexpected opportunity to reconsider the validity of this conventional description. The latter material Ta 2 NiS 5 is isostructural to the high-temperature phase of Ta 2 NiSe 5 but shows no structural phase transition, which may therefore be regarded as a simple semiconductor with a much larger band gap ( ∼ 0.25 eV at 150 K) than that of Ta 2 NiSe 5 ( ∼ 0.16 eV ) [15] . Most notably, a huge peak appears at ∼ 0.4 eV in the optical conductivity spectrum of Ta 2 NiSe 5 in a wide temperature range both below and above T c [13] , which is absent in the spectrum of Ta 2 NiS 5 . We consider the origin of this peak using two approaches: a DFT-based electronic structure calculation and a density-matrix renormalization group (DMRG) calculation [23] of an effective model. As we will discuss below, these calculations lead us to the remarkable conclusion given briefly above. We carry out the DFT-based electronic structure calculations using the wien 2k code [24] , where we use the generalized gradient approximation for electron correlations with the exchange correlation potential given in Ref. [25] . The crystal structures of the high-temperature orthorhombic phase (space group C m c m ) are taken from Ref. [26] . Because the DFT-based band calculations usually underestimate the band gap, we introduce a modified Becke-Johnson (MBJ) exchange potential [27,28] with a parameter c defined in Eq. (3) of Ref. [27] and improve this underestimation. We thereby find that the band gap opens at c > 1.2 for Ta 2 NiS 5 but an unusually large value of c > 1.63 is required to open the band gap for Ta 2 NiSe 5 . We choose a value c = 1.5 in the following calculations [29] . Details of our band calculations are given in Supplemental Material [32] . In the calculation of the optical conductivity spectra [33] , we use 5046 k points in the irreducible part of the Brillouin zone, and a broadening parameter of the spectra is set to be 0.05 eV for both interband and intraband (Drude) contributions. The real part of the optical conductivity spectra σ 1 ( ω ) for the electric field E parallel to the a and c axes is shown in Figs. 2(a) and 2(b) , respectively, for both Ta 2 NiSe 5 and Ta 2 NiS 5 . The results for E ∥ a should be compared with experimental data given in Fig. 1 of Ref. [15] , where the same labeling of the peaks α , β , γ , and δ are used, and the results for E ∥ c should be compared with experimental data given in Figs. 4.9 and 4.10 of Ref. [14] . We first find in Fig. 2(b) that the peak at ω ≃ 2 eV in the spectra of E ∥ c is well reproduced by our calculations for both Ta 2 NiSe 5 and Ta 2 NiS 5 if we assume c = 1.5 . The higher-energy spectral features are also well reproduced. We moreover find in Fig. 2(a) that the series of peaks at ω ≳ 1.2 eV in the spectra of E ∥ a labeled α , β , γ , and δ are all well reproduced by our calculations with the same value c = 1.5 . These agreements with experiment are remarkable in that the DFT-based calculations using the MBJ potential with an appropriate choice of the c value can reproduce all the high-energy spectral features very well in both materials [34] . 2 10.1103/PhysRevLett.120.247602.f2 FIG. 2. Calculated optical conductivity spectra of Ta 2 NiSe 5 (purple line) and Ta 2 NiS 5 (green line) for the electric field E parallel to (a) the crystallographic a axis and (b) the c axis. Vertical lines indicate the positions of the major peaks for Ta 2 NiSe 5 , which are labeled α , β , γ , and δ following Ref. [15] in (a). The same labels are put in (b) but have no relation to the labels in (a). However, we notice in Fig. 2 that this approach is quite poor in the description of the low-energy region ω ≲ 1.1 eV , in particular, for Ta 2 NiSe 5 ; i.e., the calculation predicts a metallic state although insulating in the experiment, and a huge peak observed at ω ≃ 0.4 eV [13] is absent in the calculated spectrum of E ∥ a . If Ta 2 NiSe 5 above T c is a simple semiconductor, just as Ta 2 NiS 5 , the low-energy peak should not appear, because the dipole transition at the lowest-energy region is prohibited [35] . On the other hand, if Ta 2 NiSe 5 is an excitonic insulator of the BCS type, it should be metallic above T c , which is not consistent with the experiment either. The origin of this peak is thus raised as an important issue, for which we need to invent the key to a solution. Larkin et al. [15] attributed the origin of this peak to the giant oscillator strength of spatially extended exciton-phonon bound states. Below, we will present a different solution. In order to consider this issue further, we adopt the 1D extended Falicov-Kimball model (a spinless two-band model), a minimum lattice model, to discuss the spin-singlet excitonic condensation [11,36] . We thereby calculate the optical conductivity spectrum, as well as the single-particle spectrum, to consider the low-energy excitations of the model and origin of the peak in the optical conductivity spectrum. The Hamiltonian reads H = - t c ∑ ⟨ i , j ⟩ ( c i † c j + H . c . ) - t f ∑ ⟨ i , j ⟩ ( f i † f j + H . c . ) + D 2 ∑ i ( c i † c i - f i † f i ) + V ∑ i c i † c i f i † f i , (1) where c i † ( f i † ) creates an electron in the conduction (valence) band orbital at site i , ⟨ i , j ⟩ indicates the nearest-neighbor pair of sites, t c and t f are the hopping integrals of c and f orbitals, respectively, assuming a direct band gap ( t c t f < 0 ), D is the level separation between c and f orbitals, and V is the interorbital Coulombic repulsion. We consider the case at half filling. We apply the dynamical DMRG method [37] to calculate the spectra, which are given by the imaginary part of the dynamical correlation functions I ( ω ) = 1 π Im ⟨ ψ 0 | A † 1 H + ω - E 0 - i η A | ψ 0 ⟩ , (2) where E 0 and | ψ 0 ⟩ are the ground-state energy and wave function, respectively, and A is the quantum operator corresponding to the physical quantity analyzed. A small real number η ( > 0 ) is introduced in the calculation to shift the poles of the correlation function into the complex plane. For the optical conductivity spectrum, we employ the dipole operator d = - e ∑ l = 1 L l ( c l † c l + f l † f l - 1 ) for A . Then, the real part of the optical conductivity σ 1 is obtained as σ ( ω ) = ω I ( ω ) . The deconvolution technique [38] is used to obtain the spectrum in the thermodynamic limit η → 0 . For the single-particle spectrum, we simply take either A = c k ( f k ) or A = c k † ( f k † ) to calculate the photoemission or inverse photoemission spectra for the conduction (valence) band orbital. Since open boundary conditions are applied here, the momentum-dependent operators are defined as c k = 2 / ( L + 1 ) ∑ l sin ( k l ) c l with quasimomentum k = π z / ( L + 1 ) for integers 1 ≤ z ≤ L . The calculated results are shown in Fig. 3 , where we find that a large asymmetric peak appears in the optical conductivity spectrum σ ( ω ) . The peak position shifts upward and the peak width broadens with increasing V . Intuitively, we can understand the presence of the peak as follows: Assume a semimetallic case in the strong-coupling limit; then the electron in the conduction band, when propagates, necessarily interacts with the electron in the valence band, and the energy of the conduction-band electron increases by V , giving rise to a peak at the energy ω ≃ V . The electron-electron repulsive interaction V acts as an electron-hole attractive interaction, so that V gives the exciton binding energy. The band gap of the size ∼ V also opens in the single-particle spectrum. Thus, the presence of the interorbital interaction is enough to yield the peak in the optical conductivity spectrum, as well as the band gap in the single-particle spectrum, irrespective of whether the long-range order of the BEC occurs or not. The energy of the peak and the size of the band-gap scale with V in the strong-coupling region, although they are much reduced in the intermediate- to weak-coupling region as shown in Fig. 3 . We should stress that this situation occurs only when the noninteracting band structure is semimetallic; when it is semiconducting, the peak vanishes, irrespective of V , unless spontaneous c - f hybridization occurs. We then immediately notice that the semimetallic situation in our model corresponds to Ta 2 NiSe 5 and the semiconducting situation in our model corresponds to Ta 2 NiS 5 . 3 10.1103/PhysRevLett.120.247602.f3 FIG. 3. Calculated optical conductivity spectra σ ( ω ) of the extended Falicov-Kimball model using an L × 2 = 100 × 2 cluster. We assume t c = 1 and t f = - 0.5 , and D is chosen to keep ⟨ c i † c i ⟩ = 0.1 for each V . The inset shows the calculated single-particle spectrum A ( k , ω ) of the same model with L × 2 = 60 × 2 and its enlargement near the Fermi level, where the broadening is η = 0.05 . This explanation of the presence of the peak in the optical conductivity spectrum, together with the opening of the band gap in the semimetallic noninteracting band structure, is very simple and straightforward, which we believe should be applicable to the low-energy physics of Ta 2 NiSe 5 , although more quantitative calculations assuming, e.g., a three-chain model with electron-phonon coupling [18] , would give an improved description. To envisage the excitonic insulator states in the entire parameter space, we present the ground-state phase diagrams of the two-chain and three-chain Hubbard models calculated in the mean-field approximation [10,19,20,32] . The results in the spin-singlet channel are shown in Fig. 4 in the parameter space of the level separation [or noninteracting band gap E g = D - 2 ( | t c | + | t f | ) ] and the interorbital repulsive interaction V . The corresponding quasiparticle band dispersions are also illustrated. For the two-chain Hubbard model [see Fig. 4(a) ], we find that the ground state in the weak-coupling regime is either a band insulator when E g > 0 or an excitonic insulator when E g < 0 , just as the conventional phase diagram indicates (see Fig. 1 ). In the strong-coupling regime, on the other hand, the excitonic insulator state of the BEC type comes out over a wide region around E g ≃ 0 . For the three-chain Hubbard model [see Fig. 4(b) ], we again find that the ground state in the weak-coupling regime is either a band insulator when E g > 0 or an excitonic insulator when E g < 0 . The latter includes the Fulde-Ferrell-Larkin-Ovchinnikov (FFLO) type of excitonic insulator state when the conduction bands are degenerate, as was discussed in Ref. [20] . In the strong-coupling regime, the excitonic insulator state of the BEC type comes out again over a wide region around E g ≃ 0 . Thus, it is not surprising that the excitonic insulator state of the BEC type appears even when E g < 0 if the interaction strength V is sufficiently large. We have argued that Ta 2 NiSe 5 is located in this parameter region. Note that the paramagnetic metallic state without excitonic orderings appears for a small V region at E g < 0 in both the two-chain and three-chain models if the Fermi surface nesting is not perfect. 4 10.1103/PhysRevLett.120.247602.f4 FIG. 4. Ground-state phase diagrams of (a) the two-chain Hubbard model with t c = t , t f = - 0.5 t , and U = 2 V and (b) the three-chain Hubbard model with t c = 0.8 eV , t f = - 0.4 eV , and U = 4 V calculated by the mean-field approximation, neglecting the Hartree shift [32] . Corresponding quasiparticle band dispersions are also illustrated schematically. Finally, let us discuss some other experiments relevant to the present study. Most important is the ARPES measurement on Ta 2 NiSe 5 [11] , which indicated that the double-peak structure of the top of the valence band appears over a wide temperature range both below and above T c , as shown in Fig. 3 of Ref. [11] . This double-peak structure was reproduced by the finite-temperature variational-cluster-approximation calculation based on the extended Falicov-Kimball model, as shown in Fig. 4 of Ref. [11] , where we note that the noninteracting band structure used is semimetallic rather than semiconducting. This semimetallic band structure, together with the strong electron-hole attraction, provided the double-peak structure at the top of the valence band. The band gap remains open at temperatures much higher than T c , so that the excitonic condensation is of the BEC type. The ARPES data on Ta 2 NiSe 5 thus reinforce the claim of the present Letter, although such an implication was not emphasized in Ref. [11] . Another relevant experiment may be a time-resolved ARPES on Ta 2 NiSe 5 , where a transient metallic phase has been observed by photoexcitation [39] . If one supposes that the photoexcited carriers screen the Coulomb interaction V in the present excitonic insulator state, without changing other parameters such as the band gap, then one may expect that the noninteracting semimetallic band structure should be observed (see Fig. 4 ), just as the obtained experimental data indicate [39] , although the results depend on the pump fluence [40] . Further experimental and theoretical studies [41] are desirable. In this context, the high-pressure experiment [42] is also interesting if one supposes that the applying pressure enhances the band overlap E g ( < 0 ) without changing the Coulomb interaction V . In summary, we studied the electronic states of an excitonic insulator candidate Ta 2 NiSe 5 and its related material Ta 2 NiS 5 using the DFT-based electronic structure calculations and the DMRG and mean-field analyses of the low-energy effective models, paying particular attention to the observed optical conductivity spectra. We showed that the spectra in the high-energy regions are described very well by the DFT-based calculations for both materials, but the description is poor for low energies. To consider the low-energy spectral features, we assumed an effective model and calculated the optical conductivity and single-particle spectra using the dynamical DMRG method. We thereby showed that the ground state of Ta 2 NiSe 5 is an excitonic insulator of the BEC type, despite the fact that the noninteracting band structure is a band-overlap semimetal. We concomitantly established a novel insulator state caused by the strong electron-hole attraction, which is a state of preformed excitons above the transition temperature with a finite band gap and may be contrasted with a Mott insulator state caused by the strong electron-electron repulsion. We thank H. Fukuyama, T. Konishi, K. Matsubayashi, T. Mizokawa, C. Monney, H. Okamura, K. Okazaki, H. Sawa, H. Takagi, and T. Toriyama for enlightening discussions. S. N. acknowledges the technical assistance of U. Nitzsche. This work was supported by Grants-in-Aid for Scientific Research (Nos. JP15H06093, JP17K05530, and JP18K13509) from JSPS of Japan and by the SFB 1143 of the Deutsche Forschungsgemeinschaft of Germany. [1] 1 N. F. Mott , Philos. Mag. 6 , 287 ( 1961 ). PHMAA4 0031-8086 10.1080/14786436108243318 [2] 2 D. Jérome , T. M. Rice , and W. Kohn , Phys. Rev. 158 , 462 ( 1967 ). PHRVAO 0031-899X 10.1103/PhysRev.158.462 [3] 3 B. I. Halperin and T. M. Rice , Rev. Mod. Phys. 40 , 755 ( 1968 ). RMPHAT 0034-6861 10.1103/RevModPhys.40.755 [4] 4 J. Kuneš , J. Phys. Condens. Matter 27 , 333201 ( 2015 ). JCOMEL 0953-8984 10.1088/0953-8984/27/33/333201 [5] 5 F. X. Bronold and H. Fehske , Phys. Rev. B 74 , 165107 ( 2006 ). PRBMDO 1098-0121 10.1103/PhysRevB.74.165107 [6] 6 K. Seki , R. Eder , and Y. Ohta , Phys. Rev. B 84 , 245106 ( 2011 ). PRBMDO 1098-0121 10.1103/PhysRevB.84.245106 [7] 7 B. Zenker , D. Ihle , F. X. Bronold , and H. Fehske , Phys. Rev. B 85 , 121102(R) ( 2012 ). PRBMDO 1098-0121 10.1103/PhysRevB.85.121102 [8] 8 A. N. Kozlov and L. A. Maksimov , Sov. Phys. JETP 21 , 790 ( 1965 ). SPHJAR 0038-5646 [9] 9 Y. Wakisaka , T. Sudayama , K. Takubo , T. Mizokawa , M. Arita , H. Namatame , M. Taniguchi , N. Katayama , M. Nohara , and H. Takagi , Phys. Rev. Lett. 103 , 026402 ( 2009 ). PRLTAO 0031-9007 10.1103/PhysRevLett.103.026402 [10] 10a T. Kaneko , T. Toriyama , T. Konishi , and Y. Ohta , Phys. Rev. B 87 , 035121 ( 2013 ); PRBMDO 1098-0121 10.1103/PhysRevB.87.035121 10b T. Kaneko , T. Toriyama , T. Konishi , and Y. Ohta Phys. Rev. B 87 , 199902 ( 2013 ). PRBMDO 1098-0121 10.1103/PhysRevB.87.199902 [11] 11 K. Seki , Y. Wakisaka , T. Kaneko , T. Toriyama , T. Konishi , T. Sudayama , N. L. Saini , M. Arita , H. Namatame , M. Taniguchi , N. Katayama , M. Nohara , H. Takagi , T. Mizokawa , and Y. Ohta , Phys. Rev. B 90 , 155116 ( 2014 ). PRBMDO 1098-0121 10.1103/PhysRevB.90.155116 [12] 12 S. Y. Kim , Y. Kim , C.-J. Kang , E.-S. An , H. K. Kim , M. J. Eom , M. Lee , C. Park , T.-H. Kim , H. C. Choi , B. I. Min , and J. S. Kim , ACS Nano 10 , 8888 ( 2016 ). ANCAC3 1936-0851 10.1021/acsnano.6b04796 [13] 13 Y. F. Lu , H. Kono , T. I. Larkin , A. W. Rost , T. Takayama , A. V. Boris , B. Keimer , and H. Takagi , Nat. Commun. 8 , 14408 ( 2017 ). NCAOBW 2041-1723 10.1038/ncomms14408 [14] 14 T. I. Larkin , PhD Thesis, University of Stuttgart , 2016 . [15] 15 T. I. Larkin , A. N. Yaresko , D. Pröpper , K. A. Kikoin , Y. F. Lu , T. Takayama , Y.-L. Mathis , A. W. Rost , H. Takagi , B. Keimer , and A. V. Boris , Phys. Rev. B 95 , 195144 ( 2017 ). PRBMDO 2469-9950 10.1103/PhysRevB.95.195144 [16] 16 S. A. Sunshine and J. A. Ibers , Inorg. Chem. 24 , 3611 ( 1985 ). INOCAJ 0020-1669 10.1021/ic00216a027 [17] 17 F. J. Di Salvo , C. H. Chen , R. M. Fleming , J. V. Waszczak , R. G. Dunn , S. A. Sunshine , and J. A. Ibers , J. Less-Common Met. 116 , 51 ( 1986 ). JCOMAH 0022-5088 10.1016/0022-5088(86)90216-X [18] 18 T. Kaneko , B. Zenker , H. Fehske , and Y. Ohta , Phys. Rev. B 92 , 115106 ( 2015 ). PRBMDO 1098-0121 10.1103/PhysRevB.92.115106 [19] 19 K. Sugimoto , T. Kaneko , and Y. Ohta , Phys. Rev. B 93 , 041105 ( 2016 ). PRBMDO 2469-9950 10.1103/PhysRevB.93.041105 [20] 20 T. Yamada , K. Domon , and Y. Ōno , J. Phys. Soc. Jpn. 85 , 053703 ( 2016 ). JUPSAU 0031-9015 10.7566/JPSJ.85.053703 [21] 21 K. Sugimoto and Y. Ohta , Phys. Rev. B 94 , 085111 ( 2016 ). PRBMDO 2469-9950 10.1103/PhysRevB.94.085111 [22] 22 H. Matsuura and M. Ogata , J. Phys. Soc. Jpn. 85 , 093701 ( 2016 ). JUPSAU 0031-9015 10.7566/JPSJ.85.093701 [23] 23 S. R. White , Phys. Rev. Lett. 69 , 2863 ( 1992 ). PRLTAO 0031-9007 10.1103/PhysRevLett.69.2863 [24] 24 P. Blaha , K. Schwarz , G. K. H. Madsen , D. Kvasnicka , and J. Luitz , WIEN2k ( Technische Universität Wien , Vienna, 2002 ). [25] 25 J. P. Perdew , K. Burke , and M. Ernzerhof , Phys. Rev. Lett. 77 , 3865 ( 1996 ). PRLTAO 0031-9007 10.1103/PhysRevLett.77.3865 [26] 26 A. Jain , S. P. Ong , G. Hautier , W. Chen , W. D. Richards , S. Dacek , S. Cholia , D. Gunter , D. Skinner , G. Ceder , and K. A. Persson , APL Mater. 1 , 011002 ( 2013 ). AMPADS 2166-532X 10.1063/1.4812323 [27] 27 F. Tran and P. Blaha , Phys. Rev. Lett. 102 , 226401 ( 2009 ). PRLTAO 0031-9007 10.1103/PhysRevLett.102.226401 [28] 28a D. Koller , F. Tran , and P. Blaha , Phys. Rev. B 83 , 195134 ( 2011 ); PRBMDO 1098-0121 10.1103/PhysRevB.83.195134 28b D. Koller , F. Tran , and P. Blaha Phys. Rev. B 85 , 155109 ( 2012 ). PRBMDO 1098-0121 10.1103/PhysRevB.85.155109 [29] Our preliminary hybrid-functional calculations [30] also predicted that Ta 2 NiS 5 is semiconducting while Ta 2 NiSe 5 is semimetallic, just as our MBJ calculations with c = 1.5 predicted. A similar result was also given for Ta 2 NiS 5 [31] . [30] 30 F. Tran and P. Blaha , Phys. Rev. B 83 , 235118 ( 2011 ). PRBMDO 1098-0121 10.1103/PhysRevB.83.235118 [31] 31 L. Li , P. Gong , W. Wang , B. Deng , L. Pi , J. Yu , X. Zhou , X. Shi , H. Li , and T. Zhai , ACS Nano 11 , 10264 ( 2017 ). ANCAC3 1936-0851 10.1021/acsnano.7b04860 [32] 32 See Supplemental Material at http://link.aps.org/supplemental/10.1103/PhysRevLett.120.247602 for details of our band structure calculations, discussion on the effects of the spin-orbit coupling, and some aspects of the theoretical models used. [33] 33 C. Ambrosch-Draxl and J. O. Sofo , Comput. Phys. Commun. 175 , 1 ( 2006 ). CPHCBZ 0010-4655 10.1016/j.cpc.2006.03.005 [34] We note that the calculations of Ref. [15] did not offer such good agreements with the experiment as ours, due perhaps to the use of different approximations and computational techniques. We point out that the inclusion of the spin-orbit coupling does not change our results significantly and that the use of the crystal structure of the low-temperature monoclinic phase of Ta 2 NiSe 5 does not modify the high-energy spectral features appreciably in agreement with the experiment [14,15] . [35] This is the case for both high-temperature orthorhombic and low-temperature monoclinic phases. [36] 36 S. Ejima , T. Kaneko , Y. Ohta , and H. Fehske , Phys. Rev. Lett. 112 , 026401 ( 2014 ). PRLTAO 0031-9007 10.1103/PhysRevLett.112.026401 [37] 37 E. Jeckelmann , Phys. Rev. B 66 , 045114 ( 2002 ). PRBMDO 0163-1829 10.1103/PhysRevB.66.045114 [38] 38 S. Nishimoto and E. Jeckelmann , J. Phys. Condens. Matter 16 , 613 ( 2004 ). JCOMEL 0953-8984 10.1088/0953-8984/16/4/010 [39] 39 K. Okazaki (unpublished). [40] 40 S. Mor , M. Herzog , D. Golež , P. Werner , M. Eckstein , N. Katayama , M. Nohara , H. Takagi , T. Mizokawa , C. Monney , and J. Stähler , Phys. Rev. Lett. 119 , 086401 ( 2017 ). PRLTAO 0031-9007 10.1103/PhysRevLett.119.086401 [41] 41 Y. Murakami , D. Golež , M. Eckstein , and P. Werner , Phys. Rev. Lett. 119 , 247601 ( 2017 ). PRLTAO 0031-9007 10.1103/PhysRevLett.119.247601 [42] 42 K. Matsubayashi , CiNii Articles, available at http://ci.nii.ac.jp/naid/110009990261/ .

PY - 2018/6/14

Y1 - 2018/6/14

N2 - We analyze the measured optical conductivity spectra using the density-functional-theory-based electronic structure calculation and density-matrix renormalization group calculation of an effective model. We show that, in contrast to a conventional description, the Bose-Einstein condensation of preformed excitons occurs in Ta2NiSe5, despite the fact that a noninteracting band structure is a band-overlap semimetal rather than a small band-gap semiconductor. The system above the transition temperature is therefore not a semimetal but rather a state of preformed excitons with a finite band gap. A novel insulator state caused by the strong electron-hole attraction is thus established in a real material.

AB - We analyze the measured optical conductivity spectra using the density-functional-theory-based electronic structure calculation and density-matrix renormalization group calculation of an effective model. We show that, in contrast to a conventional description, the Bose-Einstein condensation of preformed excitons occurs in Ta2NiSe5, despite the fact that a noninteracting band structure is a band-overlap semimetal rather than a small band-gap semiconductor. The system above the transition temperature is therefore not a semimetal but rather a state of preformed excitons with a finite band gap. A novel insulator state caused by the strong electron-hole attraction is thus established in a real material.

UR - http://www.scopus.com/inward/record.url?scp=85048562462&partnerID=8YFLogxK

UR - http://www.scopus.com/inward/citedby.url?scp=85048562462&partnerID=8YFLogxK

U2 - 10.1103/PhysRevLett.120.247602

DO - 10.1103/PhysRevLett.120.247602

M3 - Article

C2 - 29956960

AN - SCOPUS:85048562462

VL - 120

JO - Physical Review Letters

JF - Physical Review Letters

SN - 0031-9007

IS - 24

M1 - 247602

ER -