Skip to main content

Thank you for visiting You are using a browser version with limited support for CSS. To obtain the best experience, we recommend you use a more up to date browser (or turn off compatibility mode in Internet Explorer). In the meantime, to ensure continued support, we are displaying the site without styles and JavaScript.

Experimental realization of a topological crystalline insulator in SnTe


A topological insulator is an unusual quantum state of matter, characterized by the appearance, at its edges or on its surface, of a gapless metallic state that is protected by time-reversal symmetry1,2. The discovery of topological insulators has stimulated the search for other topological states protected by other symmetries3,4,5,6,7, such as the recently predicted8 topological crystalline insulator (TCI) in which the metallic surface states are protected by the mirror symmetry of the crystal. Here we present experimental evidence for the TCI phase in tin telluride (SnTe), which has been predicted to be a TCI (ref. 9). Our angle-resolved photoemission spectra show the signature of a metallic Dirac-cone surface band, with its Dirac point slightly away from the edge of the surface Brillouin zone in SnTe. Such a gapless surface state is absent in a cousin material, lead telluride, in line with the theoretical prediction.


The surface state of three-dimensional (3D) topological insulators is characterized by a spin non-degenerate Dirac-cone energy dispersion protected by time-reversal symmetry. In topological insulators, the time-reversal symmetry plays a key role in characterizing the topological properties such as the quantum spin Hall effect, the dissipation-less spin current and the magnetoelectric effect10,11,12,13. In contrast, in TCIs, the metallic surface states are protected by the mirror symmetry (reflection symmetry) of the crystal8. The TCIs are characterized by a new topological invariant called the mirror Chern number, instead of the Z2 invariant in topological insulators. Intuitively, the existence of mirror symmetry allows one to divide the Hilbert space into left and right, and considering only one of them can single out a non-trivial topology that is otherwise cancelled and undetected. Therefore, even when an insulator is trivial in the topological insulator sense, it can still be non-trivial in the TCI sense when it possesses a mirror symmetry and its mirror Chern number is non-zero8,9. Indeed, it was recently shown9 that such a situation is realized in an insulating crystal having the rock-salt structure (in which the {001}, {110} and {111} surfaces have mirror symmetry with respect to the (110) mirror plane, see Fig. 1a) when a band inversion occurs at the high-symmetry L points of the bulk Brillouin zone; intriguingly, it was further predicted9, on the basis of tight-binding calculations, that a narrow-gap IVVI semiconductor SnTe is such a TCI, whereas the isostructural PbTe is not. It is thus of particular importance to experimentally examine the possibility of the TCI phase in these semiconductors, to establish the concept of this new topological state of matter and possibly to find topological phenomena beyond the framework of known topological materials.

Figure 1: Dirac-like band dispersion in SnTe.

a, The bulk Brillouin zone (red lines) and the corresponding (001) surface Brillouin zone (blue lines). The (110) mirror plane is indicated by the green shaded area. b, ARPES intensity mapping at EF at T = 30 K for SnTe plotted as a function of the 2D wave vector measured with the He 1 line (h v = 21.2 eV); this intensity is obtained by integrating the spectra within ±10 meV of EF. c,d, Near-EF ARPES intensity measured at h ν = 21.2 eV as a function of the wave vector and EB along the cut crossing the and point (red arrows in b), respectively. e,f, Energy distribution curves (e) along the cut (yellow arrow in b) measured at h ν = 21.2 eV, and the corresponding intensity plot (f). The dashed lines in e are a guide to the eyes to trace the band dispersion. gj, ARPES intensity measured at T = 30 K with various photon energies across the cut crossing the point (green arrow in b). k, The same as in g but measured at T = 130 K. The ARPES intensity is divided by the Fermi–Dirac distribution function convoluted with the instrumental resolution. l, A slice of the bulk Brillouin zone in the (110) plane, together with the momentum points in which the ARPES data for c,d and gk were obtained; kz values were estimated by using the inner-potential value of 8.5 eV as determined by the normal-emission ARPES measurement. m, Comparison of the band dispersion for various photon energies extracted by tracking the peak position of momentum distribution curves obtained along the green arrow in b; error bars are shown for the data at h ν = 92, 83, and 21.2 eV, and they reflect the uncertainties originating from the momentum resolution and the standard deviation in the peak positions of momentum distribution curves. The h ν = 83 eV data are particularly broad at high EB, which is partly due to a mixing of the bulk band.

In our angle-resolved photoemission spectroscopy (ARPES) experiment, we paid particular attention to the momentum space around the point of the surface Brillouin zone corresponding to a projection of the L point of the bulk Brillouin zone where a direct bulk bandgap resides14,15,16 and the appearance of topological surface states is predicted9; note that the (110) mirror plane is projected to the high-symmetry line in the surface Brillouin zone (Fig. 1a). Our extensive ARPES measurements of the occupied states suggest that the bulk-band maximum is indeed located around the point (see Supplementary Fig. S1). As shown in Fig. 1b, the ARPES intensity at the Fermi level (EF) measured with the photon energy h ν = 21.2 eV on the (001) surface exhibits a bright intensity pattern centred around the point and is elongated along the direction. The band dispersion along two selected cuts (red arrows in Fig. 1b) exhibits a linearly dispersive feature crossing EF, as shown in Fig. 1c,d. The top of this Dirac-like band is located not at the point but at a point slightly away from it (called here the point), as one can infer from the band dispersion along the cut (Fig. 1e,f) showing the band maxima on both sides of the point ( and for the first and second surface Brillouin zones, respectively). Such a characteristic M-shaped dispersion is not expected from the bulk-band calculations at any kz (wave vector perpendicular to the surface) values14,15,16, but is predicted for the surface band9 (Supplementary Information), suggesting that the observed Dirac-like band originates from the surface states.

To further examine whether the Dirac-like band is of surface or bulk origin, we have carried out an ARPES measurement along the cut crossing the point for various photon energies. As one immediately recognizes in Fig. 1gj, the energy position of the band is stationary with respect to the h ν variation. In fact, when we plot the extracted dispersions for different photon energies in the same panel, they overlap each other within the experimental uncertainties of 0.05 eV (near EF) to 0.1 eV (at higher binding energy, EB), demonstrating the surface origin of the Dirac-like band. Note that the broadening of the spectra on the right-hand side of the branch at higher EB evident in Fig. 1hj is probably due to a mixture of the bulk state whose energy position changes with h ν, although the bulk state is obviously very broad and we could not clearly resolve its dispersion.

We note that, because as-grown crystals of SnTe tend to show a heavily hole-doped nature16,17,18, a key to the present observation of the Dirac-like band was to reduce hole carriers in the crystal by minimizing Sn vacancies during the growth procedure. In fact, the Dirac-like surface state was not resolved in the previous ARPES study16, mainly owing to the heavily hole-doped nature of the sample (chemical potential was located 0.5 eV lower when compared with our data). Furthermore, a downward band bending, possibly due to a loss of Te atoms on cleaving, was obviously taking place near the surface (Supplementary Information), which further worked in our favour.

As shown in Fig. 1k, the ARPES data at T = 130 K divided by the Fermi–Dirac distribution function indicate that the left- and right-hand side dispersion branches actually merge into a single peak above EF. The Dirac-point energy is estimated to be 0.05 eV above EF from a linear extrapolation of the two dispersion branches (Fig. 1m) that were determined from the peak positions in the momentum distribution curves; furthermore, the Dirac band velocities extracted from the dispersions are 4.5 and 3.0 eV Å, for the left- and right-hand side branches, respectively. One can see in Fig. 1m that the band dispersion exhibits no discernible change with temperature (compare the 30 K and 130 K data for h ν = 92 eV).

One may argue that in SnTe the well-known rhombohedral distortion19 would break the mirror symmetry with respect to the (110) plane and destroy the signature of the Dirac-cone surface states. However, one can safely exclude this possibility in the present experiment, because the rhombohedral phase transition temperature is known to be strongly dependent on the carrier density19 and in our samples the transition occurs well below 30 K (the temperature of our ARPES measurements), which is corroborated by the absence of a kink in the temperature dependence of the resistivity (see Supplementary Fig. S6). In addition, the (001) surface of the cubic structure has two mirror planes, and the rhombohedral distortion breaks the mirror symmetry of only one of those two mirror planes. This means that two of the original four Dirac cones remain gapless in the rhombohedral phase; furthermore, as the rhombohedral distortion in SnTe is weak (it induces only 1.6% displacement of the atomic positions19), the expected result is an opening of a small gap at the Dirac point in the other two Dirac cones. Therefore, the small rhombohedral distortion, even when it happens, will not significantly change the surface state spectrum.

To further elucidate the topology of the Dirac cone in detail, we have determined the whole band dispersion in the 2D momentum space. By selecting a specific photon energy (h ν = 92 eV), owing to the matrix-element effects, we found it possible to pick up the dispersion of a single Dirac cone centred at the point ( Dirac cone) while suppressing the intensity of the Dirac cone. Figure 2ae shows the near-EF ARPES intensity measured along several cuts (A–E) around the point. Along cut A (Fig. 2a), the surface band has its top at an EB of 0.45 eV. On moving from cut A to E, the band maximum (white arrow) approaches EF (cuts A–B), passes EF (cut C), and then disperses back again towards higher EB (cuts D–E). This result establishes the cone-shaped dispersion of the Dirac-like band in the 2D momentum space as in three-dimensional topological insulators1,2 and graphene20. In passing, we have surveyed electronic states throughout the Brillouin zone and found no evidence for other metallic surface states (Supplementary Fig. S1) and thus conclude that the surface electronic states consist of four Dirac cones in the first surface Brillouin zone. This indicates that this material is not a topological insulator but is a TCI owing to an even number of band-inversion points9 that is reflected in the number of Dirac cones.

Figure 2: Two-dimensional band dispersion of SnTe.

ae, Near-EF ARPES intensity for SnTe as a function of the wave vector and EB measured at h ν = 92 eV along the cuts (A–E) around the point shown by the red arrows in the surface Brillouin zone in f. The white arrow marks the top of the dispersion. f, Surface Brillouin zone and the momentum cuts of the measurement (red arrows). g, ARPES intensity mappings for SnTe in a 2D wave-vector plane at various EB values. Note that the intensity distribution for EB≥0.45 eV is strongly affected by the bulk-band contributions. h, Schematic 2D band dispersions near EF depicting the evolution of the surface Dirac cones. The blue circles show energy contours for representative EB slices, highlighting the Lifshitz transition9 (see Supplementary Information for details).

As shown in the ARPES-intensity contour plots in Fig. 2g for several EB slices, the Dirac cone in SnTe is anisotropic and slightly elongated along the direction, and its topology shows a Lifshitz transition as a function of band filling: namely, at EB = 0.15 eV the cross-section is closed and is elongated towards , but it becomes open at EB = 0.30 eV, suggesting that it is reconnected with the Dirac cone on the other side of (see Supplementary Fig. S5); at EB≥0.45 eV, the bulk band creates strong intensities and partly smears the surface state. This Lifshitz transition is interesting, because it would accompany a marked change in the Dirac-carrier properties and provide another ingredient in the physics of topological insulators. The observed evolution in the 2D band dispersion presenting a double Dirac-cone structure is schematically depicted in Fig. 2h. Although SnTe samples are always p-type, one can access the upper part of this double cone by using scanning tunnelling microscopy or field-effect-transistor devices.

To see how unique SnTe is among isostructural IVVI semiconductors, we have performed an ARPES measurement of PbTe and directly compared the near-EF electronic states around the point, as shown in Fig. 3a,b. The PbTe single crystals used here were specially tuned to be only weakly electron doped and were of very high quality, with an electron mobility of 60,000 cm2 V−1 s−1 (Supplementary Information). Intriguingly, the spectral feature of PbTe shows no evidence for the metallic Dirac-like band, and exhibits only a broad feature originated from the top of the bulk valence band21, suggesting that this material is an ordinary (trivial) insulator. Note that this broad feature is intrinsic and is not due to a bad crystallinity, because deeper bands show clear dispersions (Supplementary Information). This naturally suggests that a topological phase transition takes place in a solid-solution system Pb1−xSnxTe (Fig. 3c). This conclusion agrees with the tight-binding calculation9 that predicted that the valence bands at four L points in SnTe are inverted relative to PbTe, resulting in different mirror Chern numbers (2 versus 0). One can thus infer that the bulk bandgap closes at a critical x value, xc, accompanied by a parity change of the valence-band wavefunction and an emergence/disappearance of the Dirac-cone surface state. Therefore, the present results have established the TCI phase in SnTe, which is in contrast to the trivial nature of isostructural PbTe. Our results unambiguously demonstrate the validity of the concept of TCIs and suggests the existence of many more kinds of topological material.

Figure 3: Comparison of the band structure between SnTe and PbTe.

a, Near-EF energy distribution curves around the point for SnTe and PbTe measured with h ν = 21.2 eV; note that the energy axes are different for SnTe and PbTe. b, Corresponding ARPES-intensity plots. c, Schematic illustration of the evolution of the band dispersion in Pb1−xSnxTe expected from the present ARPES experiment. SS, CB, and VB denote the surface state, the bulk conduction band and the bulk valence band, respectively.


High-quality single crystals of SnTe and PbTe were grown by a modified Bridgeman method in sealed evacuated quartz-glass tubes from high-purity elements (Sn (99.99%), Pb (99.998%), Te (99.999%)). To obtain SnTe crystals with minimal Sn vacancy, a starting ratio of Sn/Te = 51:49 was chosen and, after melting the elements at high temperature, the tube was slowly cooled to 770 °C (which is only 20 °C below the melting point) and quenched into cold water; the carrier density estimated from the Hall coefficient was 2×1020 cm−3, which is lower than usual17,18. PbTe crystals were grown with a starting composition of Pb/Te = 1.005:1 by slowly cooling the melt from 980 °C to 700 °C at 2°C h−1 and holding at 700 °C for 12 h; the carrier density in the resulting crystals was very low at 1.7×1017 cm−3. Both SnTe and PbTe single crystals are single domain and show good crystallinity in X-ray Laue analysis, and their detailed transport properties are described in the Supplementary Information. ARPES measurements were performed with the MBS-A1 and VG-Scienta SES2002 electron analysers with a high-intensity helium discharge lamp at Tohoku University and also with tunable synchrotron lights at the beamline BL28A at the Photon Factory (KEK). To excite photoelectrons, we used the He Iα resonance line (h ν = 21.218 eV) and the circularly polarized lights of 50–100 eV at Tohoku University and the Photon Factory, respectively. The energy and angular resolutions were set at 10–30 meV and 0.2°, respectively. Samples were cleaved in situ along the (001) crystal plane in an ultrahigh vacuum of 1×10−10 torr at room temperature. A shiny mirror-like surface was obtained after cleaving the samples, confirming their high quality. The Fermi level of the samples was referenced to that of a gold film evaporated onto the sample holder.


  1. 1

    Hasan, M. Z. & Kane, C. L. Colloquium: Topological insulators. Rev. Mod. Phys. 82, 3045–3067 (2010).

    ADS  Article  Google Scholar 

  2. 2

    Qi, X-L. & Zhang, S-C. Topological insulators and superconductors. Rev. Mod. Phys. 83, 1057–1110 (2011).

    ADS  Article  Google Scholar 

  3. 3

    Schnyder, A. P., Ryu, S., Furusaki, A. & Ludwig, A. W. W. Classification of topological insulators in three spatial dimensions. Phys. Rev. B 78, 195125 (2008).

    ADS  Article  Google Scholar 

  4. 4

    Kitaev, A. Periodic table for topological insulators and superconductors. Preprint at (2009).

  5. 5

    Ran, Y. Weak indices and dislocations in general topological band structures. Preprint at (2010).

  6. 6

    Mong, R. S. K., Essin, A. M. & Moore, J. E. Antiferromagnetic topological insulators. Phys. Rev. B 81, 245209 (2010).

    ADS  Article  Google Scholar 

  7. 7

    Li, R., Wang, J., Qi, X-L. & Zhang, S-C. Dynamical axion field in topological magnetic insulators. Nature Phys. 6, 284–288 (2010).

    ADS  Article  Google Scholar 

  8. 8

    Fu, L. Topological crystalline insulators. Phys. Rev. Lett. 106, 106802 (2011).

    ADS  Article  Google Scholar 

  9. 9

    Hsieh, T. H. et al. Topological crystalline insulators in the SnTe material class. Nature Commun. 3, 982 (2012).

    Article  Google Scholar 

  10. 10

    Kane, C. L. & Mele, E. J. Z2 topological order and the quantum spin Hall effect. Phys. Rev. Lett. 95, 146802 (2005).

    ADS  Article  Google Scholar 

  11. 11

    Bernevig, B. A., Hughes, T. L. & Zhang, S-C. Quantum spin Hall effect and topological phase transition in HgTe quantum wells. Science 314, 1757–1761 (2006).

    ADS  Article  Google Scholar 

  12. 12

    Xu, C. & Moore, J. E. Stability of the quantum spin Hall effect: Effects of interactions, disorder, and Z2 topology. Phys. Rev. B 73, 045322 (2006).

    ADS  Article  Google Scholar 

  13. 13

    Qi, X-L., Hughes, T. L. & Zhang, S-C. Topological field theory of time-reversal invariant insulators. Phys. Rev. B 78, 195424 (2008).

    ADS  Article  Google Scholar 

  14. 14

    Tung, Y. W. & Cohen, M. L. Relativistic band structure and electronic properties of SnTe, GeTe, and PbTe. Phys. Rev. 180, 823–826 (1969).

    ADS  Article  Google Scholar 

  15. 15

    Melvin, J. S. & Hendry, D. C. Self-consistent relativistic energy bands for tin telluride. J. Phys. C 12, 3003–3012 (1979).

    ADS  Article  Google Scholar 

  16. 16

    Littlewood, P. B. et al. Band structure of SnTe studied by photoemission spectroscopy. Phys. Rev. Lett. 105, 086404 (2010).

    ADS  Article  Google Scholar 

  17. 17

    Richard Burke, J. Jr, Allgaier, R. S., Houston, B. B., Babiskin, J. & Siebenmann, P. G. Shubnikov-de Haas effect in SnTe. Phys. Rev. Lett. 14, 360–361 (1965).

    ADS  Article  Google Scholar 

  18. 18

    Allgaier, R. S. & Houston, B. Weak-field magnetoresistance and the valence-band structure of SnTe. Phys. Rev. B 5, 2186–2197 (1972).

    ADS  Article  Google Scholar 

  19. 19

    Iizumi, M., Hamaguchi, Y., Komatsubara, K. F. & Kato, Y. Phase transition in SnTe with low carrier concentration. J. Phys. Soc. Jpn 38, 443–449 (1975).

    ADS  Article  Google Scholar 

  20. 20

    Bostwick, A., Ohta, T., Seyller, T., Horn, K. & Rotenberg, E. Quasiparticle dynamics in graphene. Nature Phys. 3, 36–40 (2007).

    ADS  Article  Google Scholar 

  21. 21

    Nakayama, K., Sato, T., Takahashi, T. & Murakami, H. Doping induced evolution of Fermi surface in low carrier superconductor Tl-doped PbTe. Phys. Rev. Lett. 100, 227004 (2008).

    ADS  Article  Google Scholar 

Download references


We thank L. Fu for stimulating discussions. We also thank M. Komatsu, M. Nomura, E. Ieki, T. Takahashi, N. Inami, H. Kumigashira and K. Ono for their assistance in ARPES measurements, and T. Ueyama and K. Eto for their assistance in crystal growth. This work was supported by JSPS (NEXT Program and KAKENHI 23224010), JST-CREST, MEXT of Japan (Innovative Area Topological Quantum Phenomena), AFOSR (AOARD 124038) and KEK-PF (proposal number: 2012S2-001).

Author information




Y.T., T.S., K.N., S.S. and T.T. performed ARPES measurements. Z.R., K.S. and Y.A. carried out the growth of the single crystals and their characterizations. Y.T., T.S. and Y.A. conceived the experiments and wrote the manuscript.

Corresponding authors

Correspondence to T. Sato or Yoichi Ando.

Ethics declarations

Competing interests

The authors declare no competing financial interests.

Supplementary information

Supplementary Information

Supplementary Information (PDF 5500 kb)

Rights and permissions

Reprints and Permissions

About this article

Cite this article

Tanaka, Y., Ren, Z., Sato, T. et al. Experimental realization of a topological crystalline insulator in SnTe. Nature Phys 8, 800–803 (2012).

Download citation

Further reading


Quick links

Nature Briefing

Sign up for the Nature Briefing newsletter — what matters in science, free to your inbox daily.

Get the most important science stories of the day, free in your inbox. Sign up for Nature Briefing