Article | Open | Published:

# CaTe: a new topological node-line and Dirac semimetal

## Abstract

Combining first-principles calculations and effective model analysis, we predict that CaTe is a topological node-line semimetal in the absence of the spin-orbit coupling. Using a slab model, we obtain the nearly flat drumhead surface state near the Fermi level. When the spin-orbit coupling is included, three node lines will evolve into a pair of Dirac points along the MR line. These Dirac points are robust and protected by the C 4 rotation symmetry. Once this crystal symmetry is broken, the Dirac points will be eliminated, and the system becomes a strong topological insulator.

## Introduction

Topological insulator (TI) has attracted broad interest in the past 10 years.1,2,3,4,5,6,7 The unique property of TI is that it is an insulator in the bulk but has exotic metallic surface states due to the topological order. More recently, the research on topological states has been extended to three-dimensional (3D) semimetal systems.8,9,10,11,12 These systems could demonstrate many fascinating phenomena, such as Weyl fermion quantum transport and various Hall effects,13,14,15,16 consequently become the rising stars of the field. Up to now, three kinds of topological semimetals have been discovered, i.e., 3D Dirac semimetal (DSM),12,17,18,19,20,21 Weyl semimetal (WSM),8,9,22,23 and node-line semimetal (NLS).24,25,26,27,28,29 The 3D DSM has four-fold degeneracy point, which can be viewed as the kiss of two Weyl fermions with opposite chiralities in the Brillouin zone (BZ). Protected by the crystal symmetry and time reversal symmetry, 3D DSMs can be robust against external perturbations. Several materials have been theoretically predicted to be 3D DSMs12,17,18,19,20,21 and some of them have already been confirmed by experiments.30,31,32,33 If one breaks the time reversal symmetry8,22,23,34 or the inversion symmetry,35,36,37,38 the 3D DSM will evolve into WSM. Very recently, the predictions about WSM state in TaAs family37,38 have been confirmed experimentally.39,40,41,42

Unlike DSM and WSM whose band crossing points distribute at separate k points in the BZ, for a NLS the crossing points around the Fermi level form a closed loop. Several compounds have been proposed as NLSs, including Mackay-Terrones crystals,25 Bernal graphite,43 hyperhoneycomb lattices,44 and antiperovskite Cu3PdN26,27 and Cu3NZn.27 In the absence of spin-orbit coupling (SOC), time reversal symmetry together with inversion or mirror symmetry will guarantee the occurrence of node line in 3D BZ for systems with band inversion.25,26,27,37,45,46 Same with TI and WSM, NLS also has a characteristic surface state, namely, drumhead-like state.24,25,26,27,28,29 Such a 2D flat band surface state may become a route to achieve high temperature superconductivity.47,48 As a result, it is of great impetus to search new NLS.

In this study, based on first-principles calculations and effective model analysis, we propose that CaTe in CsCl-type structure is a NLS with drumhead-like surface flat bands when the SOC is ignored. As shown in Fig. 1b, around the M point, there are three node-line rings, which are perpendicular from one and another. When the SOC is included, these three node-line rings evolve into two Dirac points along the MR line. The Dirac points are robust and protected by the C 4 rotational symmetry. If this symmetry is broken, the system becomes a strong TI with Z 2 indices (1;000).

## Results and discussions

As one member of the alkaline-earth chalcogenides, CaTe has attracted tremendous interests because of its technological applications ranging from catalysis to luminescence.49,50,51,53,53 CaTe undergoes a phase transition from NaCl-type structure at ambient conditions to CsCl-type structure at hydrostatic pressure about 33 GPa.49,50 The structure of CaTe in CsCl-type is shown in Fig. 1a. The space group of this phase is $$Pm\overline{3}m$$ (NO. 221).

First, we calculate the band structure of CaTe and show the result without SOC in Fig. 2a. By checking the wave functions, we find that the valence bands and conduction bands are mainly contributed by the $$5{p}_{z}$$ (blue) state of Te and $$3{d}_{{z}^{2}}$$ (red) state of Ca, respectively, as shown in Fig. 2a. The band inversion occurs at M point, where the energy of Te-$$5{p}_{z}$$ state is higher than the energy of Ca-$$3{d}_{{z}^{2}}$$ state by about 0.75 eV. Interestingly, this kind of band inversion is not caused by the SOC, which is different from most of topological materials.1,2 We calculate the electronic structure of CaTe by applying tensile strain to check the origin of band inversion at M point. The energy difference between the Te-$$5{p}_{z}$$ state and Ca-$$3{d}_{{z}^{2}}$$ state decreases as the tensile strain increases. When the strain is larger than 5%, the band inversion at M point disappears. Therefore, the band inversion originates from the crystal field effect. With the time reversal and space inversion symmetry, such band inversion will result in node lines as proved in Weng et al.25

The effective Hamiltonian for the node line around M point can be established by using the $$\mathop{k}\limits^{\rightharpoonup }\cdot \mathop{p}\limits^{\rightharpoonup }$$ method. Considering the crystal symmetry at M point and time reversal symmetry, the effective Hamiltonian can be written as the following form:

$$H(\mathop{k}\limits^{\rightharpoonup })={g}_{0}(\mathop{k}\limits^{\rightharpoonup }){\sigma }_{0}+{g}_{x}(\mathop{k}\limits^{\rightharpoonup }){\sigma }_{x}+{g}_{z}(\mathop{k}\limits^{\rightharpoonup }){\sigma }_{z},$$

where σ x and σ z are the Pauli matrices, σ 0 is the unit matrix. $${g}_{0}(\mathop{k}\limits^{\rightharpoonup })={M}_{0}-{B}_{0}({k}_{x}^{2}+{k}_{y}^{2})-{C}_{0}{k}_{z}^{2}$$, $${g}_{x}(\mathop{k}\limits^{\rightharpoonup })=A{k}_{x}{k}_{y}{k}_{z}$$, $${g}_{z}(\mathop{k}\limits^{\rightharpoonup })={M}_{z}-$$ $${B}_{z}({k}_{x}^{2}+{k}_{y}^{2})-{C}_{z}{k}_{z}^{2}$$. This system has both the time reversal symmetry and the inversion symmetry, thus the component σ y is zero.25 The eigenvalues of this 2 × 2 effective Hamiltonian are $$E(\mathop{k}\limits^{\rightharpoonup })={g}_{0}(\mathop{k}\limits^{\rightharpoonup })\pm \sqrt{{g}_{x}^{2}(\mathop{k}\limits^{\rightharpoonup })+{g}_{z}^{2}(\mathop{k}\limits^{\rightharpoonup })}$$. When $${g}_{x}(\mathop{k}\limits^{\rightharpoonup })\mathrm{=0}$$ and $${g}_{z}(\mathop{k}\limits^{\rightharpoonup })\mathrm{=0}$$, the nodal line will emerge. It can be easily checked that the equation $${g}_{z}(\mathop{k}\limits^{\rightharpoonup })\mathrm{=0}$$ has solution only when M z B z  > 0 and M z C z  > 0. Note that such conditions apply also for the band inversion. On the other hand, $${g}_{x}(\mathop{k}\limits^{\rightharpoonup })\mathrm{=0}$$ confines the node lines in three mutually perpendicular planes (namely, k x  = 0, k y  = 0, and k z  = 0 planes ) as illustrated in Fig. 1b. Due to the fact that $${g}_{0}(\mathop{k}\limits^{\rightharpoonup })$$ does not equal to 0, which breaks the electron-hole symmetry, the node lines have finite energy dispersion.

When the SOC is considered, however, three node lines evolve into two Dirac points at the MR line as shown in Fig. 2b. At M point, the two states near the Fermi level belong to irreducible representation $${\Gamma }_{7}^{-}$$ and $${\Gamma }_{6}^{+}$$, respectively. While along the MX line, two bands have the same irreducible representation (Γ5) as shown in Fig. 2b, they can hybridize with each other, opening a small gap (about 50 meV). For both the Γ−M line and the MM′ line, the two bands around the Fermi level also belong to the same irreducible representation, thus there is no band crossing along the Γ−M line and the MM′ line. We point out here that since the band splitting is determined by the SOC, one therefore can achieve the NLS by doping the light atoms such as Se, S.

Along the MR line, which reserves the C 4 rotation symmetry, the two states with $${\Gamma }_{7}^{-}$$ and $${\Gamma }_{6}^{+}$$ at M point evolve into Γ7 and Γ6. Consequently, the hybridization between these two bands is forbidden, generating a Dirac point as shown in Fig. 2b. When the C 4 rotational symmetry is broken, e.g., by strain effect, the band crossing point will disappear, and this 3D DSM will become a strong TI with topological indices Z 2 to be (1;000).

To better understand the band inversion at M point and the topological property of this system, we derive a low-energy effective Hamiltonian at M point based on the projection-operator method.20 The M point has the D 4h symmetry and also the time reversal symmetry. As discussed above, at M point, $${\Gamma }_{7}^{-}$$ symmetry state has angular momentum j z  = ±3/2 and $${\Gamma }_{6}^{+}$$ symmetry state has angular momentum j z  = ±1/2. Therefore using the basis of ($$\left|{j_{z}}=-{\frac{1}{2}}\right\rangle _{d},\left|{j_{z}}=+{\frac{1}{2}}\right\rangle _{d},\left|{j_{z}}=-{\frac{3}{2}}\right\rangle _{p},\left|{j_{z}}=+{\frac{3}{2}}\right\rangle _{p}$$), the effective Hamiltonian around M point can be written as (see Supplementary information (S1) for details):

$${H}_{eff}= \quad\quad\quad\quad\quad\quad\quad\quad\quad\quad\quad\quad\quad\quad\quad\quad\quad\quad\quad\quad\quad\quad\quad\quad \\ \left(\begin{array}{cccc}{M}_{1}(\mathop{k}\limits^{\rightharpoonup }) & 0 & A{k}_{+}+B(\mathop{k}\limits^{\rightharpoonup }) & D(\mathop{k}\limits^{\rightharpoonup })\\ 0 & {M}_{1}(\mathop{k}\limits^{\rightharpoonup }) & {D}^{\ast }(\mathop{k}\limits^{\rightharpoonup }) & -A{k}_{-}-{B}^{\ast }(\mathop{k}\limits^{\rightharpoonup })\\ A{k}_{-}+{B}^{\ast }(\mathop{k}\limits^{\rightharpoonup }) & D(\mathop{k}\limits^{\rightharpoonup }) & {M}_{2}(\mathop{k}\limits^{\rightharpoonup }) & 0\\ {D}^{\ast }(\mathop{k}\limits^{\rightharpoonup }) & -A{k}_{+}-B(\mathop{k}\limits^{\rightharpoonup }) & 0 & {M}_{2}(\mathop{k}\limits^{\rightharpoonup }),\end{array}\right)$$

where $${M}_{1}(\mathop{k}\limits^{\rightharpoonup })={M}_{10}+{M}_{11}({k}_{x}^{2}+{k}_{y}^{2})+{M}_{12}{k}_{z}^{2}$$, $${M}_{2}(\mathop{k}\limits^{\rightharpoonup })={M}_{20}+$$ $${M}_{21}({k}_{x}^{2}+{k}_{y}^{2})+{M}_{22}{k}_{z}^{2}$$, $$B(\mathop{k}\limits^{\rightharpoonup })={B}_{1}{k}_{+}{k}_{z}^{2}+ {B}_{2}({k}_{x}^{3}+i{k}_{y}^{3})+i{B}_{3}{k}_{-}{k}_{x}{k}_{y}$$, $$D(\mathop{k}\limits^{\rightharpoonup })={D}_{1}({k}_{x}^{2}-{k}_{y}^{2}){k}_{z}+i{D}_{2}{k}_{x}{k}_{y}{k}_{z}$$, k ± = k x  ± ik y . Along the k z axis (where k x  = 0, k y  = 0), the effective Hamiltonian is diagonal, and the eigenvalues are $$E(\mathop{k}\limits^{\rightharpoonup })={M}_{1}(\mathop{k}\limits^{\rightharpoonup })$$ and $$E(\mathop{k}\limits^{\rightharpoonup })={M}_{2}(\mathop{k}\limits^{\rightharpoonup })$$. As mentioned above, the Dirac point is on the MR line, thus it is interesting to discuss the effective model along this line. Since there is the band inversion between $${\left|{j}_{z}=\pm \frac{1}{2}\right\rangle }_{d}$$ and $${\left|{j}_{z}=\pm \frac{3}{2}\right\rangle }_{p}$$ at M point, it is easy to obtain that M 10 < M 20, M 22 < 0 < M 12, and the Dirac points locate at $${\mathop{k}\limits^{\rightharpoonup }}_{c}=(\frac{\pi }{a},\frac{\pi }{a},{k}_{zc}=\pm \sqrt{\frac{{M}_{20}-{M}_{10}}{{M}_{12}-{M}_{22}}})$$. Neglecting the high-order terms, $$E({\mathop{k}\limits^{\rightharpoonup }}_{c}+\mathop{\delta k}\limits^{\rightharpoonup })$$ can be expressed as $$({M}_{12}+{M}_{22}){k}_{zc} \\ \\ \delta {k}_{z}\pm \sqrt{{({M}_{12}-{M}_{22})}^{2}{k}_{zc}^{2}\delta {k}_{z}^{2}+{A}^{2}(\delta {k}_{x}^{2}+\delta {k}_{y}^{2})}$$, where δk x,y,z are the small displacements from $${\mathop{k}\limits^{\rightharpoonup }}_{c}$$. In the vicinity of $${\mathop{k}\limits^{\rightharpoonup }}_{c}$$, the band dispersion is linear, thus our effective Hamiltonian describes exactly the 3D massless Dirac fermions.

The band inversion at M point and the Dirac nodes in CaTe suggest the existence of topological nontrivial surface state. Figure 3a, b shows the surface state of CaTe (001) surface without/with the SOC, respectively. When the SOC is absent, the system is a NLS, and possesses nearly flat surface band around the Fermi energy. As shown in Fig. 3a, our numerical results find that the nearly flat surface “drumhead” state appears in the interiors of the projected nodal line rings on the (001) surface around the $$\overline{M}$$ point. Since the slab we used has two surfaces, there are two surface states as shown in the red lines in the Fig. 3a. The particle-hole symmetry is broken by the non-zero term $${g}_{0}(\mathop{k}\limits^{\rightharpoonup })$$, thus these two surface bands are not perfectly flat with about 70 meV bandwidth. This type of 2D flat bands is proposed as a novel route to achieve high temperature superconductivity.47,48

When the SOC is included, three node lines are gapped out and evolve into a pair of Dirac points along the MR line, thus the NLS becomes a 3D DSM. There is a bulk Dirac node projected on the $$\overline{M}$$ point (the red dot) as shown in Fig. 3b. Along the $$\overline{M}-\overline{X}$$, there is also a projected bulk Dirac node, which locates near the $$\overline{X}$$ point denoted by red dots. Figure 3b clearly shows the gapped bulk states along the $$\overline{\Gamma }-\overline{X}$$ direction and the existence of surface Dirac cones (in the blue circle) due to the topologically nontrivial Z 2 indices, same as the case of Na3Bi18 and Cd3As2.19

In summary, based on the first-principles calculations and effective model analysis, we suggest that CaTe in CsCl-type structure is a NLS when the SOC is ignored. There are three node-line rings that are perpendicular from one and another around M point. With band inversion at M point, this NLS is protected by the time reversal symmetry and space inversion symmetry. When the SOC is included, three node-line rings become a pair of Dirac points. These Dirac nodes are robust and protected by the C 4 crystal symmetry and the system becomes a DSM. Experimentally, to achieve the NLS state, one may consider to decrease the SOC effect by doping the light atoms such as Se, S into the system.The simple cubic structure of CaTe makes this compound much easier synthesized. On the other hand, the clean Fermi surface of CaTe results in a simple surface state, which brings benefit to the measurement of flat-band surface state. Therefore, CaTe is a promising candidate material of NLS.

## Methods

The electronic band structure calculations have been carried out using the full potential linearized augmented plane-wave method as implemented in the WIEN2K package.54 To obtain accurate band inversion strength and band order, the modified Becke-Johnson exchange potential together with the local-density approximation for the correlation potential (MBJLDA) has been applied.55 We also check the electronic structure with other exchange potentials like the local-density approximation Perdew-Burke-Ernzerhof parametrization of the generalized gradient approximation.56 The results show no significant differences. The plane-wave cutoff parameter R MT K max is set to be 7 and a 16 × 16 × 16 mesh is used for the BZ integral. The SOC is treated using the second-order variational procedure.

To study the surface states in CaTe, we use a 200-unit-cells-thick (001) slab with the top (bottom) surface terminated by Ca (Te) atoms. The surface state is then calculated using the tight-binding method. The hopping parameters are determined from the maximally localized Wannier functions,57 which are projected from the Bloch state derived from the first-principles calculations.

## References

1. 1

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

2. 2

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

3. 3

Kane, C. L. & Mele, E. J. Quantum spin hall effect in graphene. Phys. Rev. Lett. 95, 226801 (2005).

4. 4

Kane, C. L. & Mele, E. J. Z 2 topological order and the quantum spin hall effect. Phys. Rev. Lett. 95, 146802 (2005).

5. 5

Bernevig, B. A. & Zhang, S. C. Quantum spin hall effect. Phys. Rev. Lett. 96, 106802 (2006).

6. 6

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).

7. 7

Zhang, H. et al. Topological insulators in Bi 2 Se 3, Bi 2 Te 3 and Sb 2 Te 3 with a single Dirac cone on the surface. Nat. Phys. 5, 438–442 (2009).

8. 8

Wan, X. G., Turner, A. M., Vishwanath, A. & Savrasov, S. Y. Topological semimetal and Fermi-arc surface states in the electronic structure of pyrochlore iridates. Phys. Rev. B 83, 205101 (2011).

9. 9

Balents, L. Viewpoint: Weyl electrons kiss. Physics 4, 36 (2011).

10. 10

Ando, Y. Topological insulator materials. J. Phys. Soc. Jpn. 82, 102001 (2013).

11. 11

Yang, K. Y., Lu, Y. M. & Ran, Y. Quantum hall effects in a Weyl semimetal: possible application in pyrochlore iridates. Phys. Rev. B 84, 075129 (2011).

12. 12

Wehling, T. O., Black-Schaffer, A. M. & Balatsky, A. V. Dirac materials. Adv. Phys. 63, 1–76 (2014).

13. 13

Hosur, P. & Qi, X. L. Recent developments in transport phenomena in Weyl semimetals. Compt. Rend. Phys. 14, 857–870 (2013).

14. 14

Zyuzin, A. A. & Burkov, A. A. Topological response in Weyl semimetals and the chiral anomaly. Phys. Rev. B 86, 115133 (2012).

15. 15

Vazifeh, M. M. & Franz, M. Electromagnetic response of Weyl semimetals. Phys. Rev. Lett. 111, 027201 (2013).

16. 16

Parameswaran, S. A., Grover, T., Abanin, D. A., Pesin, D. A. & Vishwanath, A. Probing the chiral anomaly with nonlocal transport in three-dimensional topological semimetals. Phys. Rev. X 4, 031035 (2014).

17. 17

Young, S. M. et al. Dirac semimetal in three dimensions. Phys. Rev. Lett. 108, 140405 (2012).

18. 18

Wang, Z. et al. Dirac semimetal and topological phase transitions in A 3 Bi (A=Na, K, Rb). Phys. Rev. B 85, 195320 (2012).

19. 19

Wang, Z., Weng, H. M., Wu, Q., Dai, X. & Fang, Z. Three-dimensional Dirac semimetal and quantum transport in Cd 3 As 2. Phys. Rev. B 88, 125427 (2013).

20. 20

Du, Y. et al. Dirac and Weyl semimetal in XYBi (X=Ba, Eu; Y=Cu, Ag and Au). Sci. Rep. 5, 14423 (2015).

21. 21

Gibson, Q. D. et al. Three-dimensional Dirac semimetals: design principles and predictions of new materials. Phys. Rev. B 91, 205128 (2015).

22. 22

Xu, G., Weng, H. M., Wang, Z., Dai, X. & Fang, Z. Chern semimetal and the quantized anomalous hall effect in HgCr 2 Se 4. Phys. Rev. Lett. 107, 186806 (2011).

23. 23

Burkov, A. A. & Balents, L. Weyl semimetal in a topological insulator multilayer. Phys. Rev. Lett. 107, 127205 (2011).

24. 24

Burkov, A. A., Hook, M. D. & Balents, L. Topological nodal semimetals. Phys. Rev. B 84, 235126 (2011).

25. 25

Weng, H. et al. Topological node-line semimetal in three-dimensional graphene networks. Phys. Rev. B 92, 045108 (2015).

26. 26

Yu, R., Weng, H., Fang, Z., Dai, X. & Hu, X. Topological node-line semimetal and Dirac semimetal state in antiperovskite Cu 3 PdN. Phys. Rev. Lett. 115, 036807 (2015).

27. 27

Kim, Y., Wieder, B. J., Kane, C. L. & Rappe, A. M. Dirac line nodes in inversion-symmetric crystals. Phys. Rev. Lett. 115, 036806 (2015).

28. 28

Yang, S. Y., Pan, H. & Zhang, F. Dirac and Weyl superconductors in three dimensions. Phys. Rev. Lett. 113, 046401 (2014).

29. 29

Chen, Y. P. et al. Nanostructured carbon allotropes with Weyl-like loops and points. Nano Lett. 15, 6974–6978 (2015).

30. 30

Jeon, S. et al. Landau quantization and quasiparticle interference in the three-dimensional Dirac semimetal Cd 3 As 2. Nat. Mater. 13, 851–856 (2014).

31. 31

Neupane, M. et al. Observation of a three-dimensional topological Dirac semimetal phase in high-mobility Cd 3 As 2. Nat. Commun. 5, 3786 (2014).

32. 32

Liu, Z. K. et al. Discovery of a three-dimensional topological Dirac semimetal, Na 3 Bi. Science 343, 864–867 (2014).

33. 33

Liu, Z. K. et al. A stable three-dimensional topological Dirac semimetal Cd 3 As 2. Nat. Mater. 13, 677–681 (2014).

34. 34

Wan, X., Vishwanath, A. & Savrasov, S. Y. Computational design of Axion insulators based on 5d spinel compounds. Phys. Rev. Lett. 108, 146601 (2012).

35. 35

Halasz, G. B. & Balents, L. Time-reversal invariant realization of the Weyl semimetal phase. Phys. Rev. B 85, 035103 (2012).

36. 36

Liu, J. & Vanderbilt, D. Weyl semimetals from noncentrosymmetric topological insulators. Phys. Rev. B 90, 155316 (2014).

37. 37

Weng, H. M., Fang, C., Fang, Z., Bernevig, B. A. & Dai, X. Weyl semimetal phase in noncentrosymmetric transition-metal monophosphides. Phys. Rev. X 5, 011029 (2015).

38. 38

Huang, S. M. et al. A Weyl Fermion semimetal with surface Fermi arcs in the transition metal monopnictide TaAs class. Nat. Commun. 6, 7373 (2015).

39. 39

Lv, B. Q. et al. Experimental discovery of Weyl semimetal TaAs. Phys. Rev. X 5, 031013 (2015).

40. 40

Lv, B. Q. et al. Observation of Weyl nodes in TaAs. Nat. Phys. 11, 724–727 (2015).

41. 41

Xu, S. Y. et al. Discovery of a Weyl fermion semimetal and topological Fermi arcs. Science 349, 613–617 (2015).

42. 42

Xu, S. Y. et al. Discovery of a Weyl fermion state with Fermi arcs in niobium arsenide. Nat. Phys. 11, 748–754 (2015).

43. 43

Mikitik, G. P. & Sharlai, Y. V. Band-contact lines in the electron energy spectrum of graphite. Phys. Rev. B 73, 235112 (2006).

44. 44

Mullen, K., Uchoa, B. & Glatzhofer, D. T. Line of Dirac nodes in hyperhoneycomb lattices. Phys. Rev. Lett. 115, 026403 (2015).

45. 45

Xie, L. S. et al. A new form of Ca 3 P 2 with a ring of Dirac nodes. . APL Mater. 3, 083602 (2015).

46. 46

Zeng, M., et al. Topological semimetals and topological insulators in rare earth monopnictides. Preprint at https://arxiv.org/abs/1504.03492 (2015).

47. 47

Heikkila, T. T. & Volovik, G. E. Flat bands as a route to high-temperature superconductivity in graphite. Preprint at https://arxiv.org/abs/1504.05824 (2015).

48. 48

Kopnin, N. B., Heikkila, T. T. & Volovik, G. E. High-temperature surface superconductivity in topological flat-band systems. Phys. Rev. B 83, 220503 (2011).

49. 49

Zimmer, H. G., Winzen, H. & Syassen, K. High-pressure phase transitions in CaTe and SrTe. Phys. Rev. B 32, 4066–4070 (1985).

50. 50

Luo, H., Greene, R. G., Ghandehari, K., Li, T. & Ruoff, A. L. Structural phase transformations and the equations of state of calcium chalcogenides at high pressure. Phys. Rev. B 50, 16232–16237 (1994).

51. 51

Dadsetani, M. & Pourghazi, A. Optical properties of strontium monochalcogenides from first principles. Phys. Rev. B 73, 195102 (2006).

52. 52

Boucenna, S. et al. High pressure induced structural, elastic and electronic properties of Calcium Chalcogenides CaX (X = S, Se and Te) via first-principles calculations. Comput. Mater. Sci. 68, 325–334 (2013).

53. 53

Varshneya, D., Rathore, V., Kinge, R. & Singh, R. K. High-pressure induced structural phase transition in alkaline earth CaX (X = S, Se and Te) semiconductors: NaCl-type (B1) to CsCl-type (B2). J. Alloys Compd. 484, 239–245 (2009).

54. 54

Blaha, P., Schwarz, K., Madsen, G. K. H., Kvasnicka, D., & Luitz, J. in WIEN2K: An Augmented Plane Wave + Local Orbitals Program for Calculating Crystal Properties (ed Schwarz, K.) (Vienna University of Technology, 2001).

55. 55

Tran, F. & Blaha, P. Accurate band gaps of semiconductors and insulators with a semilocal exchange-correlation potential. Phys. Rev. Lett. 102, 226401 (2009).

56. 56

Perdew, J. P., Burke, K. & Ernzerhof, M. Generalized gradient approximation made simple. Phys. Rev. Lett. 77, 3865–3868 (1996).

57. 57

Marzari, N., Mostofi, A. A., Yates, J. R., Souza, I. & Vanderbilt, D. Maximally localized Wannier functions: theory and applications. Rev. Mod. Phys. 84, 1419–1475 (2012).

## Acknowledgements

The work was supported by the National Key Project for Basic Research of China (Grant No. 2014CB921104), NSFC under Grants No. 11525417, 11374147, 51572085. The project is also funded by Priority Academic Program Development of Jiangsu Higher Education Institutions. S.S. was supported by NSF DMR (Grant No. 1411336). Y.D. is supported by the program B for Outstanding Ph.D. candidate of Nanjing University.

### Author contributions

X.W. notices the line node and Dirac points in this system. Y.D. performs the first-principles calculations. Y.D., F.T., and D.W. do the symmetry analysis and the model. X.W. interprets the numerical results and writes the paper. All authors contribute to editing the manuscript.

### Competing interests

The authors declare no competing financial interests.

## Author information

### Affiliations

1. #### National Laboratory of Solid State Microstructures and Department of Physics, Nanjing University, Nanjing, 210093, China

• Yongping Du
• , Feng Tang
• , Di Wang
• , Li Sheng
•  & Xiangang Wan
2. #### Collaborative Innovation Center of Advanced Microstructures, Nanjing University, Nanjing, 210093, China

• Li Sheng
•  & Xiangang Wan

• Er-jun Kan
4. #### Key Laboratory of Polar Materials and Devices, Ministry of Education, East China Normal University, Shanghai, 200062, China

• Chun-Gang Duan
5. #### Department of Physics, University of California, Davis, One Shields Avenue, Davis, CA, 95616, USA

• Sergey Y. Savrasov

### Corresponding author

Correspondence to Xiangang Wan.

## Electronic supplementary material

### DOI

https://doi.org/10.1038/s41535-016-0005-4

• ### Emergence of Topological insulator and Nodal line semi-metal states in XX′Bi (X = Na, K, Rb, Cs; X′ = Ca, Sr)

• Chiranjit Mondal
• , C. K. Barman
• , Sourabh Kumar
• , Aftab Alam
•  & Biswarup Pathak

Scientific Reports (2019)

• ### Observation of Dirac-like energy band and ring-torus Fermi surface associated with the nodal line in topological insulator CaAgAs

• Daichi Takane
• , Kosuke Nakayama
• , Seigo Souma