# Hidden-symmetry-protected topological insulator in a cubic lattice

###### Abstract

Usually topological insulators are protected by time reversal symmetry. Here, we present a new type of topological insulators in a cubic lattice which is protected by a novel hidden symmetry, while time reversal symmetry is broken. The hidden symmetry has a composite antiunitary operator consisting of fractional translation, complex conjugation, sublattice exchange, and local gauge transformation. Based on the hidden symmetry, we define the hidden-symmetry polarization and topological invariant to characterize the topological insulators. The surface states have band structures with odd number of Dirac cones, where pseudospin-momentum locking occurs. When the hidden-symmetry-breaking perturbations are added on the boundaries, a gap opens in the surface band structure, which confirms that the topological insulator and the surface states are protected by the hidden symmetry. We aslo discuss the realization and detection of this new kind of topological insulator in optical lattices with ultracold atom techniques.

## I Introduction

Recently, topological phases in condensed matters attract much attention of physicistsHasan and Kane (2010); Qi and Zhang (2011). Before 1980s, it was believed that matter is classified by symmetries according to Laudau’s theory. The discovery of the quantum Hall effect overturned that belief since two distinct quantum Hall insulators may have the same symmetryKlitzing et al. (1980). Very soon, it was realized that quantum Hall insulators are classified by a topological invariant, i.e., the Chern number, which is directly related to the quantized Hall conductivityThouless et al. (1982). Thus, quantum Hall insulators are time-reversal-symmetry-breaking topological phases due to the existence of magnetic field. Since then, the door of the study of topological phases in condensed matter physics was opened. Later, the discoveries of topological insulators in two and three dimensions significantly boom the research on topological phases in condensed matter physicsKane and Mele (2005a, b); Bernevig and Zhang (2006); Bernevig et al. (2006); König et al. (2007); Fu et al. (2007); Moore and Balents (2007); Roy (2009); Fu and Kane (2007); Hsieh et al. (2008); Xia et al. (2009); Zhang et al. (2009); Chen et al. (2009); Hsieh et al. (2009a, b). In general, the topological insulators are induced by spin-orbit coupling and protected by time reversal symmetry. Such nontrivial phases are characterized by the topological edge or surface states, which exhibit spin-momentum locking.

Besides time-reversal-symmetry-protected topological insulators, there are also topological insulators protected by spatial symmetry (i.e. topological crystalline insulators) that have been predicted theoretically and prepared experimentallyFu (2011); Hsieh et al. (2012); Liu et al. (2014). Recently, we found a kind of hidden symmetry which protects the degeneracies at Dirac points of a square latticeHou (2013, 2014). This kind of hidden symmetry is a composite antiunitary symmetry, generally consisting of fractional translation, complex conjugation, sublattice exchange, and local gauge transformation. We have found a two-dimensional optical lattice preserving this kind of hidden symmetry, which supports quantum pseudospin Hall effect, i.e., a two-dimensional topological insulatorHou and Chen (2016). A natural question is whether the hidden symmetry supports the existence of topological insulators in three dimensions. In this paper, we will give a positive answer.

In the following sections, we propose a tight-binding model in a cubic lattice, which preserves a hidden symmetry, i.e., a composite antiunitary symmetry. Based on the hidden symmetry, the pseudospin, symmetry-polarization and topological invariant are defined. We calculate the dispersion relation of the system and find that the band inversions happen when changing the parameters across some fixed values. Based on the topological invariants and band inversions, the phase diagram is drawn. We evaluate the surface states of a slab geometry and calculate the pseudospin textures of the surface states. The insulator with non-trivial topological invariant has odd number of Dirac cones in the surface band structure, which have pseudospin-momentum-locking pseudospin textures. When the hidden-symmetry-breaking perturbations are added on the boundaries of the slab, a gap opens at the surface Dirac points and the surface states on the two opposite boundaries mix, even turn into bulk states when the perturbations are strong enough, which confirm that the topological insulator is protected by the hidden symmetry. The recent development of experimental techniques of ultracold atoms in optical lattices have make them become a platform to simulate the exotic physics in condensed mattersJaksch and Zoller (2005); Bloch et al. (2008); Lewenstein et al. (2007). Thus, we suggest to realize this model with ultracold atoms in optical lattices and to detect the topological properties with state-of-the-art techniques in cold atomic physics.

## Ii Model

Here, we consider two-level atoms trapped in a cubic optical lattice as shown in Fig.1(a), where the arrows represent the hopping-accompanying phases. Due to the appearing of the hopping-accompanying phases, the translation symmetry is broken. Thus, the lattice is divided into two sublattices, i.e. sublattices and , denoted by the red and blue spheres in Fig.1(a), respectively. Taking the distance between the nearest lattice sites as the unit of length, we define the primitive lattice vectors as , , and . The primitive reciprocal lattice vectors are , , and and the corresponding Brillouin zone is shown in Fig.1(b). The system can be described by the tight-binding Hamiltonian with

(1) | |||||

and

(2) | |||||

and

(3) |

where and are the two-component annihilation operators destructing an atom at a lattice site of sublattice and , respectively; represent the Pauli matrices in the color space spanned by the two atomic levels; and represent the amplitudes of hopping between the nearest lattice sites and between the next-nearest lattice sites, respectively; is the magnitude of an effective Zeeman term.

After the Fourier transformation, the Bloch Hamiltonian is obtained as

(4) | |||||

where represents a mass term. Diagonalizing Eq.(4), we arrive at the dispersion relation as

(5) |

From the dispersion relation, it is found that the energy bands are two-fold degenerate for the conduction and valence bands. When Hamiltonians and disappear, the mass term vanishes and the conduction and valence bands touched at the points and in the Brillouin zone as shown in Figs.2(a) and (b). When and appear, the mass term is non-zoro, then a gap opens between the conduction and valence bands as shown in Figs.2(c)-(d). The masses at the Dirac points have different signs for different parameter ranges as shown in Table 1. Based on the signs of masses at the Dirac points, they can be divided into eight parameter ranges: (i) , (ii) and , (iii) , (iv) and , (v) , (vi) and , (vii) , (viii) and . These insulators are classified by a topological invariant, which will be defined in Section IV. As one crosses the boundary between two neighboring parameter ranges, a band inversion happens at one of Dirac points, which indicates a topological phase transition. That is to say, the insulators in two neighboring parameter ranges belong to two distinct topological sectors. The insulators with odd number of negative masses at the Dirac points are topologically non-trivial insulators, while the ones with even number of negative masses at the Dirac points are trivial insulators, which will be confirmed in the succeeding sections of the paper. Therefore, the system is a topological insulator in parameter ranges (ii) (iv), (vi) and (viii) and is a trivial band insulator in parameter ranges (i), (iii), (v) and (vii) as shown in Fig.3.

Parameter ranges | |||||

(i) | |||||

(ii) | |||||

(iii) | |||||

(vi) | |||||

(v) | |||||

(vi) | |||||

(vii) | |||||

(viii) |

## Iii Hidden symmetry

It is easy to verify that the system has a hidden symmetry with the symmetry operator as

(6) |

where is the complex conjugate operator, is a translation operator that moves the lattice by a unit along the direction, is the Pauli matrix representing sublattice exchange, is the unit matrix in the color space, and is a local gauge transformation and is the -component of the space coordinate. The Bloch functions are supposed to have the form in the coordinate representation. The symmetry operator acts on the Bloch function as follows

(7) |

Because is the symmetry operator of the system, must be a Bloch function of the system. Thus, we obtain , and with . Thus, one can find that the symmetry operator acts on the wave vector as

If , where is a reciprocal lattice vector, then we can say that is a -invariant point in momentum space. There are eight distinct -invariant points as , , and in the Brillouin zone as shown in Fig.1(b). From Eq.(6), we obtain that the square of the hidden symmetry operator is , which has the representation based on the Bloch functions as . Therefore, we have at points while at points and in the Brillouin zone. Furthermore, since is an antiunitary operator, there must exist two-fold degeneracies at points , which are protected by the hidden symmetry Hou (2013).

## Iv topological invariant

Based on the hidden symmetry , we can define a topological invariant, which is used to classify the insulator phases of the system. The Bloch functions of the occupied bands can be written as , where is the the cell-periodic eigenstate of the Bloch Hamiltonian . The Berry connection matrix is defined as

(8) |

For the hidden symmetry , we also define a matrix as

(9) |

where is the wave vector by acting on , i.e., . Since is satisfied at -invariant points and is an antiunitary operator, it is easy to verify that is an antisymmetric matrix at the -invariant degenerate points .

For the present model with half filling, there are two occupied bands, which compose the pair bands. For the occupied pair bands, we define the charge polarization in terms of the Berry connection as

(10) |

where the integration is along the red lines on the and planes of the Brillouin zone as shown in Fig.4; is defined as ; The signs denote the and planes, respectively; for the plane and for the plane. For each occupied band, the partial charge polarization is defined as

(11) |

For the pair bands, we can also define the polarization as

(12) | |||||

The Hilbert space can be classified into two groups depending on the difference between the polarizations on the and planes,

(13) |

The polarization is an interger and only defined modulo due to the ambiguity of the log. The argument of the log has only two values associated with the even and odd values of , respectively. Therefore, we can rewrite Eq.(13) as

(14) |

The topological invariant can be defined as modulo . When is odd or even, the system is a topological insulator or a trivial band insulator. Therefore, Eq.(14) gives a distinct definition of the topological invariant.

## V Surface states and their pseudospin textures

Generally, topological insulators have special surface states, for example, the surface bands have odd number of Dirac cones in the corresponding surface Brillouin zone. Here, in order to manifest the surface states of the hidden-symmetry-protected topological insulator, we investigate a slab with open boundaries along the direction. Based the numerical results, it is found that there exists a single Dirac cone on the surface Brillouin zone for the topological insulator phases, which as shown in Fig.5 and Fig.6 for parameter ranges (ii) and (iv), respectively. In the these two parameter ranges, the system is a topological insulator but the location of the surface Dirac point in the surface Brillouin zone are different. In parameter range (ii), the surface Dirac point locates at points of the surface Brillouin zone as shown in Fig.5(a), while, in parameter range (iv), the surface Dirac point locates at point of the surface Brillouin zone as shown Fig.6(a). For every state on the surface Dirac cone, the distribution of probability density concentrate on one of the open boundaries as shown in Fig.5(b) and Fig.6(b). The Dirac cone surface states are two-fold degenerate, since they localize the opposite boundaries of the slab. When the quantum states are outside of the Dirac cone, they become bulk states, that is to say, the surface states only occur on the Dirac cone area of the surface Brillouin zone.

In order to investigate the pseudospin texture of the surface states, we define the pseudospin operators as , , and with the commutation relations . For the surface states, the pseudospins form a vortex or antivortex pseudospin texture on the surface Brillouin zone with a number number or , respectively. For the case in the parameter range (ii), Fig.5(c) shows the pseudospin texture of the average pseudospin components on the surface Brillouin zone and Fig.5(d) shows that the average pseudospin component is vanishing for the Dirac surface states. That is to say, there is a singularity at the surface Dirac points for the pseudospin texture. Integrating the Berry connection along a circle enclosed the Dirac point for a valence band surface state, one can obtain a Berry phase, which can be used to define a winding number , so the pseudospin form an anti-vortex structure. For the case in parameter range (iv), Fig.6(c) and Fig.6(d) show the pseudospin texture of the average pseudospin components on the surface Brillouin zone and the average pseudospin component , respectively. Similarly, the only the in-plane pseudospin components exist and they form a vortex. The different point is that the vortex has a opposite winding number , compared with the case in the parameter range (ii). Beside the parameter ranges (ii) and (iv), the parameter ranges (vi) and (viii) also support the existence of topological insulators. The Dirac points have the same position and the surface states have the same pseudospin texture on the surface Brillouin zone for the parameter ranges (ii) and (vi), and for the parameter ranges (iv) and (viii), respectively.

## Vi The effects of the hidden-symmetry-breaking perturbations

Since the topological insulator and the surface states are protected by the hidden symmetry , the surface states should be gapped if some perturbations breaking the hidden symmetry are added on the boundaries of the lattice. In order to verify the protection by hidden symmetry , we add the hidden-symmetry-breaking perturbation terms on the two open boundaries of a slab and investigate the effects of these terms. We assume that the hidden-symmetry-breaking perturbations on the boundaries has the form,

(15) |

where is the magnitude of the perturbations; and denote the boundary surfaces of sublattice and . We calculate the dispersion relations, probability densities, and pseudospin textures for , , and , , , which are shown in Fig.7 and Fig.8, respectively. Fig.7(a) and Fig.8(a) show the highest valence bands and the lowest conduction bands, which correspond to the surface states in the case without hidden-symmetry-breaking perturbations. It is found that the hidden-symmetry-breaking perturbations open a gap between the highest valence and lowest conduction energy bands and the Dirac cones in the surface Brillouin zone disappear. Fig.7(b) and Fig.8(b) show the probability density profiles of the highest valence states with the wave vectors and , respectively, from which it is found that the mixing between the surface states on the two opposite boundaries happens due to the existence of the hidden-symmetry-breaking perturbations. Fig.7(c) and Fig.8(c) show the pseudospin textures of the highest valence states, which seem to manifest similar vortex pseudospin textures as the case without hidden-symmetry-breaking perturbations. In fact, for the case with hidden-symmetry-breaking perturbations, the out-of-plane pseudospin component appears as shown in Fig.7(d) and Fig.8(d), so the singularity of pseudospin texture disappears and the pseudospin textures are not vortices, which are consistent with the disappearing of the Dirac cones. The above characters confirm that the topological insulator and the surface states are protected by the hidden symmetry .

## Vii Experimental techniques for realization and detection of the topological insulators with ultracold atoms in optical lattices

During recent years, ultracold atoms in optical lattices have become a platform to simulate the exotic physics in condensed matters, especially some of which are difficult to realize in real solid materialsJaksch and Zoller (2005); Bloch et al. (2008); Lewenstein et al. (2007). A lot of experimental techniques have been developed to construct various optical lattices, such as laser-assisting tunnelingAidelsburger et al. (2011, 2013); Miyake et al. (2013); Wu et al. (2016), shaking optical latticeStruck et al. (2012, 2013). Due to the advantage of ultracold atoms in optical lattices, they have often employed to explore the physics of topological phasesGoldman et al. (2016, 2009, 2010); Liu et al. (2010); Kennedy et al. (2013); Bermudez et al. (2010); Béri and Cooper (2011). All of the techniques provide a foundation to design a model to realize a three-dimensional hidden-symmetry-protected topological insulator in optical lattices.

In order to realize the model of Eqs.(1), (2), and (3), we select two hyperspin states of cold atoms Li or K to be trapped in an cubic optical lattice formed by three pairs of lasers. These two hyperspin states can be regarded as the basis of the color space. The hyperspin-switching hopping can be induced by fine-designed Raman laser fieldsAidelsburger et al. (2011, 2013); Miyake et al. (2013); Wu et al. (2016). The accompanying phases of hopping can be realized by tuning the directions and frequencies of assistant lasersChen et al. (2017).

There also many techniques to detect the topological properties in optical lattices. The atomic interferometry is a very useful technique to measure a relative phase. Based on this technique, a direct measurement of the Zak phase in topological Bloch bands was performedAtala et al. (2013) and an Aharonov-Bohm interferometer was constructed for determining Bloch band topologyDuca et al. (2015). The concrete schemes were designed to measure Chern numberAbanin et al. (2013) and topological invariant Grusdt et al. (2014) with atomic interferometry. Very recently, Bloch state tomography was developed to detect Berry curvature and topological invariants, including single- and multiband Chern and numbersLi et al. (2016). Another detecting technique is Bragg spectroscopyStamper-Kurn et al. (1999), which can be employed to probe the dispersion relation of optical lattice. A scheme to detect the edge states based on Bragg scattering was proposedGoldman et al. (2012). The edge states can also be detected by direct imaging methodGoldman et al. (2013). The high-resolution uorescence imaging can probe optical lattices at single-site levelBakr et al. (2010); Sherson et al. (2010), so it can be employed to detect edge or surface states by measuring populations of atoms. Based on the above detecting techniques, it is feasible that the topological invariant and the surface states in the hidden-symmetry-protected topological insulators are measured and detected.

## Viii Conclusion

In summary, we have studied a tight-binding model in a cubic lattice that preserves a hidden symmetry, which has a composite antiunitary operator consisting of fractional translation, complex conjugation, sublattice exchange, and local gauge transformation. Based on the hidden symmetry, we defined a topological invariant which classifies the insulator phases of the lattice. In some parameter ranges, the lattice supports a non-trivial topological insulator protected by the hidden symmetry. For the hidden-symmetry-protected topological insulator, the surface states localized on one of open boundaries and have a single Dirac cone band structure on the surface Brillouin zone. We also defined pseudospin operators and find that the surface states have only in-plane components, which form a vortex or antivortex pseudospin texture having a winding number , respectively. When additional hidden-symmetry-breaking perturbations on the open boundaries of a slab geometry are added, an energy gap opens between the highest valance and lowest conduction bands and the surface states on the two opposite boundaries mix, even turn into bulk states when the perturbations are strong enough. Furthermore, the out-of-plane pseudospin component appears and the singularity of pseudospin texture vanishes. The results of the case with additional hidden-symmetry-breaking perturbations demonstrate that the topological insulator and surface states are protected by the hidden symmetry .

###### Acknowledgements.

This work was supported by the National Natural Science Foundation of China under Grants No. 11274061 (J.M.H.) and No. 11504171 (W.C.). W.C. was also supported by the Natural Science Foundation of Jiangsu Province in China under Grant No. BK20150734.## References

- Hasan and Kane (2010) M. Z. Hasan and C. L. Kane, “Colloquium: Topological insulators,” Rev. Mod. Phys. 82, 3045 (2010).
- Qi and Zhang (2011) X.-L. Qi and S.-C. Zhang, “Topological insulators and superconductors,” Rev. Mod. Phys. 83, 1057 (2011).
- Klitzing et al. (1980) K. v. Klitzing, G. Dorda, and M. Pepper, “New method for high-accuracy determination of the fine-structure constant based on quantized Hall resistance,” Phys. Rev. Lett. 45, 494 (1980).
- Thouless et al. (1982) D. J. Thouless, M. Kohmoto, M. P. Nightingale, and M. den Nijs, “Quantized Hall conductance in a two-dimensional periodic potential,” Phys. Rev. Lett. 49, 405 (1982).
- Kane and Mele (2005a) C. L. Kane and E. J. Mele, “Quantum spin Hall effect in graphene,” Phys. Rev. Lett. 95, 226801 (2005a).
- Kane and Mele (2005b) C. L. Kane and E. J. Mele, “ topological oder and the qantum spin Hall effect,” Phys. Rev. Lett. 95, 146802 (2005b).
- Bernevig and Zhang (2006) B. A. Bernevig and S.-C. Zhang, “Quantum spin hall effect,” Phys. Rev. Lett. 96, 106802 (2006).
- Bernevig et al. (2006) B. A. Bernevig, T. L. Hughes, and S.-C. Zhang, “Quantum spin hall effect and topological phase transition in hgte quantum wells,” Science 314, 1757 (2006).
- König et al. (2007) M. König, S. Wiedmann, C. Brüne, A. Roth, H. Buhmann, L. W. Molenkamp, X.-L. Qi, and S.-C. Zhang, “Quantum spin hall insulator state in hgte quantum wells,” Science 318, 766 (2007).
- Fu et al. (2007) L. Fu, C. L. Kane, and E. J. Mele, “Topological insulators in three dimensions,” Phys. Rev. Lett. 98, 106803 (2007).
- Moore and Balents (2007) J. E. Moore and L. Balents, “Topological invariants of time-reversal-invariant band structures,” Phys. Rev. B 75, 121306 (2007).
- Roy (2009) R. Roy, “Topological phases and the quantum spin Hall effect in three dimensions,” Phys. Rev. B 79, 195322 (2009).
- Fu and Kane (2007) L. Fu and C. L. Kane, “Topological insulators with inversion symmetry,” Phys. Rev. B 76, 045302 (2007).
- Hsieh et al. (2008) D. Hsieh, D. Qian, L. Wray, Y. Xia, Y. S. Hor, R. J. Cava, and M. Z. Hasan, “A topological Dirac insulator in a quantum spin Hall phase,” Nature 452, 970 (2008).
- Xia et al. (2009) Y. Xia, et al., “Observation of a large-gap topological-insulator class with a single Dirac cone on the surface,” Nat. Phys. 5, 398 (2009).
- Zhang et al. (2009) H. Zhang, C.-X. Liu, X.-L. Qi, X. Dai, Z. Fang, and S.-C. Zhang, “Topological insulators in BiSe, BiTe and SbTe with a single Dirac cone on the surface,” Nat. Phys. 5, 438 (2009).
- Chen et al. (2009) Y. L. Chen, et al., “Experimental realization of a three-dimensional topological insulator, BiTe,” Science 325, 178 (2009).
- Hsieh et al. (2009a) D. Hsieh, et al., “A tunable topological insulator in the spin helical Dirac transport regime,” Nature 460, 1101 (2009a).
- Hsieh et al. (2009b) D. Hsieh, et al., ‘‘Observation of time-reversal-protected single-Dirac-cone topological-insulator states in and ,” Phys. Rev. Lett. 103, 146401 (2009b).
- Fu (2011) L. Fu, “Topological crystalline insulators,” Phys. Rev. Lett. 106, 106802 (2011).
- Hsieh et al. (2012) T. H. Hsieh, H. Lin, J. Liu, W. Duan, A. Bansil, and L. Fu, “Topological crystalline insulators in the SnTe material class,” Nat. Commun. 3, 982 (2012).
- Liu et al. (2014) C.-X. Liu, R.-X. Zhang, and B. K. VanLeeuwen, “Topological nonsymmorphic crystalline insulators,” Phys. Rev. B 90, 085304 (2014).
- Hou (2013) J.-M. Hou, “Hidden-symmetry-protected topological semimetals on a square lattice,” Phys. Rev. Lett. 111, 130403 (2013).
- Hou (2014) J.-M. Hou, “Moving and merging of Dirac points on a square lattice and hidden symmetry protection,” Phys. Rev. B 89, 235405 (2014).
- Hou and Chen (2016) J.-M. Hou and W. Chen, “Hidden-symmetry-protected quantum pseudo-spin Hall effect in optical lattices,” Phys. Rev. A 93, 063626 (2016).
- Jaksch and Zoller (2005) D. Jaksch and P. Zoller, “The cold atom Hubbard toolbox,” Ann. Phys. 315, 52 (2005).
- Bloch et al. (2008) I. Bloch, J. Dalibard, and W. Zwerger, “Many-body physics with ultracold gases,” Rev. Mod. Phys. 80, 885 (2008).
- Lewenstein et al. (2007) M. Lewenstein, A. Sanpera, V. Ahufinger, B. Damski, A. Sen, and U. Sen, “Ultracold atomic gases in optical lattices: mimicking condensed matter physics and beyond,” Adv. Phys. 56, 243 (2007).
- Aidelsburger et al. (2011) M. Aidelsburger, M. Atala, S. Nascimbène, S. Trotzky, Y.-A. Chen, and I. Bloch, “Experimental realization of strong effective magnetic fields in an optical lattice,” Phys. Rev. Lett. 107, 255301 (2011).
- Aidelsburger et al. (2013) M. Aidelsburger, M. Atala, M. Lohse, J. T. Barreiro, B. Paredes, and I. Bloch, “Realization of the Hofstadter hamiltonian with ultracold atoms in optical lattices,” Phys. Rev. Lett. 111, 185301 (2013).
- Miyake et al. (2013) H. Miyake, G. A. Siviloglou, C. J. Kennedy, W. C. Burton, and W. Ketterle, “Realizing the Harper hamiltonian with laser-assisted tunneling in optical lattices,” Phys. Rev. Lett. 111, 185302 (2013).
- Wu et al. (2016) Z. Wu, L. Zhang, W. Sun, X.-T. Xu, B.-Z. Wang, S.-C. Ji, Y. Deng, S. Chen, X.-J. Liu, and J.-W. Pan, “Realization of two-dimensional spin-orbit coupling for Bose-Einstein condensates,” Science 354, 83 (2016).
- Struck et al. (2012) J. Struck, C. Ölschläger, M. Weinberg, P. Hauke, J. Simonet, A. Eckardt, M. Lewenstein, K. Sengstock, and P. Windpassinger, “Tunable gauge potential for neutral and spinless particles in driven optical lattices,” Phys. Rev. Lett. 108, 225304 (2012).
- Struck et al. (2013) J. Struck, et al., “Engineering ising-XY spin-models in a triangular lattice using tunable artificial gauge fields,” Nat. Phys. 9, 738 (2013).
- Goldman et al. (2016) N. Goldman, J. C. Budich, and P. Zoller, “Topological quantum matter with ultracold gases in optical lattices,” Nat. Phys. 12, 639 (2016).
- Goldman et al. (2009) N. Goldman, A. Kubasiak, A. Bermudez, P. Gaspard, M. Lewenstein, and M. A. Martin-Delgado, “Non-abelian optical lattices: Anomalous quantum Hall effect and Dirac fermions,” Phys. Rev. Lett. 103, 035301 (2009).
- Goldman et al. (2010) N. Goldman, I. Satija, P. Nikolic, A. Bermudez, M. A. Martin-Delgado, M. Lewenstein, and I. B. Spielman, “Realistic time-reversal invariant topological insulators with neutral atoms,” Phys. Rev. Lett. 105, 255302 (2010).
- Liu et al. (2010) G. Liu, S.-L. Zhu, S. Jiang, F. Sun, and W. M. Liu, “Simulating and detecting the quantum spin Hall effect in the kagome optical lattice,” Phys. Rev. A 82, 053605 (2010).
- Kennedy et al. (2013) C. J. Kennedy, G. A. Siviloglou, H. Miyake, W. C. Burton, and W. Ketterle, “Spin-orbit coupling and quantum spin Hall effect for neutral atoms without spin flips,” Phys. Rev. Lett. 111, 225301 (2013).
- Bermudez et al. (2010) A. Bermudez, L. Mazza, M. Rizzi, N. Goldman, M. Lewenstein, and M. A. Martin-Delgado, “Wilson fermions and axion electrodynamics in optical lattices,” Phys. Rev. Lett. 105, 190404 (2010).
- Béri and Cooper (2011) B. Béri and N. R. Cooper, “ topological insulators in ultracold atomic gases,” Phys. Rev. Lett. 107, 145301 (2011).
- Chen et al. (2017) W. Chen, H.-Z. Lu, and J.-M. Hou, “Topological semimetals with a double-helix nodal link,” Phys. Rev. B 96, 041102 (2017).
- Atala et al. (2013) M. Atala, M. Aidelsburger, J. T. Barreiro, D. Abanin, T. Kitagawa, E. Demler, and I. Bloch, “Direct measurement of the Zak phase in topological Bloch bands,” Nat. Phys. 9, 795 (2013).
- Duca et al. (2015) L. Duca, T. Li, M. Reitter, I. Bloch, M. Schleier-Smith, and U. Schneider, “An Aharonov-Bohm interferometer for determining Bloch band topology,” 347, 288 (2015).
- Abanin et al. (2013) D. A. Abanin, T. Kitagawa, I. Bloch, and E. Demler, “Interferometric approach to measuring band topology in 2D optical lattices,” Phys. Rev. Lett. 110, 165304 (2013).
- Grusdt et al. (2014) F. Grusdt, D. Abanin, and E. Demler, “Measuring topological invariants in optical lattices using interferometry,” Phys. Rev. A 89, 043621 (2014).
- Li et al. (2016) T. Li, L. Duca, M. Reitter, F. Grusdt, E. Demler, M. Endres, M. Schleier-Smith, I. Bloch, and U. Schneider, “Bloch state tomography using Wilson lines,” Science 352, 1094 (2016).
- Stamper-Kurn et al. (1999) D. M. Stamper-Kurn, A. P. Chikkatur, A. Görlitz, S. Inouye, S. Gupta, D. E. Pritchard, and W. Ketterle, “Excitation of phonons in a Bose-Einstein condensate by light scattering,” Phys. Rev. Lett. 83, 2876 (1999).
- Goldman et al. (2012) N. Goldman, J. Beugnon, and F. Gerbier, “Detecting chiral edge states in the Hofstadter optical lattice,” Phys. Rev. Lett. 108, 255303 (2012).
- Goldman et al. (2013) N. Goldman, J. Dalibard, A. Dauphin, F. Gerbier, M. Lewenstein, P. Zoller, and I. B. Spielman, “Direct imaging of topological edge states in cold-atom systems,” Proc. Natl. Acad. Sci. U.S.A. 110, 6736 (2013).
- Bakr et al. (2010) W. S. Bakr, A. Peng, M. E. Tai, R. Ma, J. Simon, J. I. Gillen, S. Fölling, L. Pollet, and M. Greiner, “Probing the superfluid-to-Mott insulator transition at the single-atom level,” Science 329, 547 (2010).
- Sherson et al. (2010) J. F. Sherson, C. Weitenberg, M. Endres, M. Cheneau, I. Bloch, and S. Kuhr, “Single-atom-resolved fluorescence imaging of an atomic Mott insulator,” Nature. 467, 68 (2010).