Unconventional superconductivity in YPtBi and related topological semimetals

Unconventional superconductivity in YPtBi and related topological semimetals

Markus Meinert meinert@physik.uni-bielefeld.de Center for Spinelectronic Materials and Devices, Bielefeld University, D-33501 Bielefeld, Germany
July 13, 2019
Abstract

YPtBi, a topological semimetal with very low carrier density, was recently found to be superconducting below  K. In the conventional theory, the nearly vanishing density of states around the Fermi level would imply a vanishing electron-phonon coupling and would therefore not allow for superconductivity. Based on relativistic density functional theory calculations of the electron-phonon coupling in YPtBi it is found that carrier concentrations of more than  cm are required to explain the observed critical temperature with the conventional pairing mechanism, which is several orders of magnitude larger than experimentally observed. It is very likely that an unconventional pairing mechanism is responsible for the superconductivity in YPtBi and related topological semimetals with the Half-Heusler structure.

A series of Half-Heusler compounds with heavy elements were predicted to have topologically non-trivial band order Lin2010 (); Al-Sawei2010 (); Feng2010 (). These compound have high cubic symmetry, however without inversion symmetry. The normal band order with the -like, twofold degenerate state sitting above the -like, fourfold degenerate -state is inverted in some of these compounds due to spin-orbit coupling. In their natural state, the cubic symmetry leads to a band degeneracy at around the Fermi level, rendering them semimetals with topologically non-trivial band order (topological semimetals) and very low density of states (DOS) at the Fermi level . By breaking the cubic symmetry with some amount of uniaxial strain, the compounds can be made insulating, so they could become 3D topological insulators Qi2011 (). They would exhibit metallic surface states with Dirac-like dispersion, i.e., the electrons behave as massless particles with ultrahigh mobility, while at the same time being insulating in the bulk. These surface states are topologically protected as long as time-reversal symmetry is preserved, i.e., they are protected against scattering from non-magnetic impurities. Indeed, for some of these materials there is experimental evidence for topologically nontrivial bandstructures and the presence of Dirac surface states Liu2011 (); Shekhar2012 (); Nowak2015 (), although none were found to be insulating in the bulk. Some compounds from this class were found to be superconductors with critical temperatures up to 1.8 K, e.g. LaPtBi, LuPtBi, LuPdBi, YPtBi, YPdBi Goll2008 (); Shekhar2013 (); Tafti2013 (); Xu2014 (); Nakajima2015 (). Compounds of the type PdBi ( is a lanthanide with an open shell) that show coexisiting local moment antiferromagnetism as well as superconductivity were found, pointing to the presence of spin triplet Cooper pairs Nakajima2015 (), which is allowed due to the missing structural inversion symmetry Sigrist2007 (). Due to the topologically nontrivial band structure, novel collective excitations are possible, in particular surface Majorana fermions Sato2009 (). These could provide the basis for low-decoherence quantum processing Leijnse2012 ().

Superconducting semiconductors such as GeTe and SnTe are long known Hein1964 (); Allen1969 () and their superconductivity can be explained Allen1969 () with the Eliashberg theory of electron-phonon mediated superconductivity. SrTiO, the most dilute semiconductor known to date, has and its superconductivity can not be explained by simple electron-phonon coupling Schooley1965 (); Bustarret2015 (). Instead, a plasmon-assisted mechanism was proposed to explain the unusual dependence of on the carrier density Takada1980 (). From the BCS theory the well-known expression for the superconducting transition temperature is obtained, where is a cutoff frequency, that is often identified with the Debye frequency, and is the effective interaction potential. Thus, the critical temperature is expected to increase with increasing . This expectation was confirmed for GeTe and SnTe, but in these materials is limited to a few hundred mK Allen1969 (). More recently, superconductivity just below was discovered in highly B doped diamond Ekimov2004 () and in CuBiSe Hor2010 (), a prototype topological insulator for . For the latter case, it was shown by first principles calculations of the electron-phonon coupling that the conventional pairing mechanism is most likely not strong enough to give rise to the rather high observed critical temperature Zhang2015 (). Furthermore, the possibility of superconductivity in the surface states of topological insulators was explored recently DasSharma2013 (); Li2014 (), and it was shown that surface electron-phonon interaction can be strong.

Naturally the question arises whether the superconductivity in the topological Half-Heusler compounds is of the conventional, phonon-mediated type. To shed some light on this question, first principles calculations of the electron-phonon coupling for a topological semimetal from the Half-Heusler class are presented here. The compound YPtBi was chosen as a representative member of this class, which is a bulk superconductor with a critical temperature of  K Butch2011 (); Bay2012 (); Shekhar2013 (); Bay2014 ().

The calculations were carried out with the Quantum Espresso distribution QE () within the framework of density functional theory (DFT). Relativistic PAW potentials DalCorso2010 () (including spin-orbit coupling, SOC) from the PSlibrary DalCorso2014 () were employed with kinetic energy cutoffs of 40 Ry for the wavefunctions and 400 Ry for the charge density. The results were checked against all-electron calculations including SOC with the full potential linearized augmented plane-wave (FLAPW) method with the elk code elk () and were found to agree very well. The Perdew-Burke-Ernzerhof (PBE) generalized gradient approximation (GGA) was used for the exchange-correlation energy and potential. Since YPtBi is a semimetal, the use of a semilocal potential to describe the band structure is justified. The dynamical matrices and electron-phonon matrix elements with phonon mode index and band indices were obtained with density functional perturbation theory on a -point mesh and -point mesh. Electron-phonon coupling was calculated applying an interpolation scheme described in Ref. Wierzbowska2005, . The Eliashberg spectral function

(1)

was evaluated on -point and -point meshes. The spectral function was obtained for several widths of a Gaussian approximation for the -function between 0.004 and 0.02 Ry. The resulting density of states and electron-phonon coupling constant , where

(2)

were extrapolated with a linear fit to the limit. Convergence tests suggest that the accuracy for is of the order . The superconducting gap was calculated by solving the isotropic Eliashberg equations self-consistently as a function of temperature with a routine implemented in the elk code elk (), which is based on a similar algorithm as described in Ref. Margine2013, . The critical temperature was obtained by interpolating with cubic splines and finding the inflection point. Additionally, the McMillan-Allen-Dynes formula

(3)

with the logarithmic average phonon frequency and the screened Coulomb pseudopotential was evaluated for comparison Allen1975 (). The Coulomb pseudopotential is usually taken as a parameter of the order , which we set to zero for the evaluation of the Eliashberg equations and the McMillan-Allen-Dynes equation, i.e. Coulomb repulsion is completely neglected. Thus, the critical temperatures obtained here are upper bounds for the electron-phonon induced superconductivity. Doping was treated in a rigid-band approximation by adding or subtracting electrons from the band structure and compensating for this by adding a homogeneous background charge. The experimental lattice constant of 6.65 Å was used in all calculations. In systems with very low Fermi energy (), vertex corrections should in principle be included, which were shown to increase to some extent Takada1993 (). However, for all carrier densities considered here we have , so the Eliashberg equations are expected to properly describe the electron-phonon interaction in YPtBi.

Figure 1: (a) Density of states (DOS), (b) atom-projected density of states (PDOS), (c) band structure, and (d) Fermi surface of YPtBi obtained from FLAPW calculations. DOS plots obtained from the relativistic PAW (thin gray) and FLAPW (thick red) calculations are compared in (a) to show the equivalence of the two methods.

For an accurate description of the electron-phonon coupling, we need to make sure that the calculated band structure close to is in agreement with the observed one. In the following, the computed electronic properties will be compared to experimental data to assess the validity of the band structure calculations. In Figure 1 the DOS, atom-projected DOS, band structure along high-symmetry lines and the Fermi surface are plotted. The relativistic PAW and FLAPW calculations are in excellent agreement, establishing that the PAW method with the potentials from the PSlibrary gives reliable results for YPtBi. The band structure plot clarifies that YPtBi has weakly overlapping bands close to the Brillouin zone center, making it a semimetal. The Fermi surface consists of two hole pockets and two sets of electron pockets, which belong to the fourfold degenerate representation Feng2010 (). As shown in Ref. Feng2010 (), the states lie below , so that the band order is topologically nontrivial. The hole pockets are of approximately cubic shape centered around the zone center with corners along the path. The inner hole pocket has a complex concave-convex shape and touches the outer hole pocket on the and paths. The electron pockets form a set of cigar-shaped ellipsoids with eightfold symmetry along the paths. The small Fermi surface is in agreement with the small density of states at the Fermi energy of . The calculated agrees very well with the value obtained from a heat capacity measurement, Pagliuso1999 ().

The Fermi surface obtained for YPtBi is remarkably similar to the Fermi surface of LaPtBi Oguchi2001 (). The Fermi vector in direction is and the volume enclosed by the two hole pockets is approximately . The corresponding carrier density is . Recently, Shubnikov-de Haas (SdH) oscillations in YPtBi single crystals with the magnetic field along the direction were observed with a frequency of Butch2011 (), indicating that the true Fermi surface cross section is even three times smaller than the calculated one. For the latter, a frequency of SdH oscillations with a periodicity of is expected. Thus, the dip of the conduction band minimum below the valence band maximum on the path is in fact not as deep as calculated. A beating node in the measurement indicates that there are two similar-sized Fermi surfaces contributing to the SdH oscillations, in perfect agreement with the band structure calculation. Simultaneous Hall effect measurements were analyzed with a one-band model giving . Based on the observed cross section of the Fermi surface and assuming cubic shape, one obtains an enclosed charge density of , which agrees nicely with the Hall effect measurement, however neglecting multiband effects, different mobilities and carrier compensation. This result supports that the true Fermi surface is much smaller than the calculated one. The surface-averaged effective masses on the calculated Fermi surface are and for the hole and electron pockets, respectively, where is the free-electron mass. The hole effective mass is roughly in agreement with the value extracted from SdH oscillation, Butch2011 (). In conclusion, the DFT electronic structure calculation with the PBE functional reproduces the experimental observations very well up to a small error in the overlap between conduction and valence bands. Thus, the calculated electronic structure provides a solid foundation for the evaluation of the electron-phonon coupling discussed in the following.

Figure 2: Phonon density of states (a) and derived heat capacity (b) of pristine YPtBi.

The phonon density of states and heat capacity of YPtBi are shown in Figure 2. A clear separation of acoustic and optical modes is visible. From the low-temperature part of the heat capacity a Debye temperature of is obtained, in good agreement with the experimental value of Pagliuso1999 (). Because of the small Fermi surface, only very short -vectors with can connect different parts of the surface, which gives rise to the scattering of an electron state into another. Thus, the electron-phonon coupling is limited to a small region close to the zone center. From the extrapolation scheme for the Brillouin zone integration is obtained, obviously at the limit of the numerical accuracy of the Brillouin zone sampling. Certainly is small, but a more accurate will require an unfeasibly dense -point mesh. With the solution of the Eliashberg equations shows that  K, much smaller than the observed critical temperature of .

Figure 3: (a) Density of states as a function of the energy. Open circles mark the values for which electron-phonon calculations were done. (b) Density of states and Fermi energy shift as a function of additional electrons per primitive cell . (c) and (d) Electron-phonon coupling constant , interaction potential , Debye temperature and Sommerfeld coefficient as functions of . (e) Calculated critical temperatures from numerical solution of the Eliashberg equations and from the McMillan-Allen-Dynes formula.

To investigate the effect of doping, electron-phonon coupling was evaluated for doping levels of electrons per primitive cell. The dynamical matrices were recomputed for each doping level, so that phonons were treated at full self-consistency with respect to doping. The corresponding densities of states and Fermi energy shifts are given in Fig. 3 (a) and (b). Because of the low DOS close to in the undoped YPtBi, small doping levels already give rise to large Fermi energy shifts. With increasing doping of both electron- or hole-type, is increased as seen in Fig. 3 (e), however electron doping () is clearly more effective. The coupling leads to a renormalization of the phonon frequencies, which is indicated by the reduction of the Debye temperature, Fig. 3 (d). This also indicates that YPtBi could be dynamically unstable at strong doping.

The observed critical temperature of is obtained at  cm or  cm with , see Fig. 3 (e). These concentrations are lower bounds, since decreases with . As seen in Fig. 3 (e), the McMillan-Allen-Dynes formula closely resembles the full numerical solution of the Eliashberg equations and remains valid down to  K. In all cases, the BCS expression for the superconducting gap, is approximately fulfilled by the numerical solutions. Also, the usual relation of with the renormalization function was found to be fulfilled in all cases, demonstrating the consistency of the Eliashberg calculations.

To study the influence of , the electron-phonon interaction potential is given in Fig. 3 (c). Over the full range of doping concentrations the interaction potential is , so the low value of for weakly and undoped YPtBi comes mainly from the low , or, equivalently, from the small Fermi surface area. These doping levels could be realized through off-stoichiometry (YPtBi crystals are mostly grown out of Bi flux, so additional Bi could easily be incorporated), or locally due to site-swap between neighboring cells. Also grain boundaries and other inhomogeneities with different stoichiometry could serve as sources of intrinsic doping. However, the carrier concentrations required for the electron-phonon coupling to be strong enough to explain the observed critical temperature are at least one order of magnitude larger than the typically observed carrier concentrations in YPtBi and three orders of magnitude larger than for the samples with lowest observed carrier concentration ( cm, Ref. Butch2011, ). Because of the increase in the Sommerfeld coefficient of the heat capacity, would increase to values around (see Fig. 3 (d)), much larger than the measured value Pagliuso1999 (). Experiments with high-quality samples indicate that the normal-state electronic properties of YPtBi are perfectly in agreement with the calculation for the ideal, undoped case Butch2011 (); Bay2012 (). A diamagnetic screening fraction around 70% was observed in the superconducting state, underlining that a large part of the material is in the superconducting state and thereby ruling out the possibility of grain-boundary superconductivity Bay2014 () or surface superconductivity DasSharma2013 (). The calculated critical temperature in the experimentally observed carrier concentration range of  cm to  cm Butch2011 (); Bay2012 (); Shekhar2013 (); Bay2014 () is  K. However, an even more remarkable observation is that the experimental critical temperature of YPtBi varies little across different samples despite the carrier concentrations vary over two orders of magnitude. From Fig. 3 (e) one would expect a variation of over several orders of magnitude in that range.

The lack of a clear correlation between normal-state electronic properties, sample quality, and critical temperature indicates that electron-phonon interaction induced by doping is not an explanation for the superconductivity in YPtBi. The relation between critical field and temperature observed in Ref. Bay2012, deviates from conventional -wave behavior and suggests that the material could be a -wave superconductor, very similar to CuBiSe. On the other hand, Cooper pair wave functions with angular orbital momentum are not protected by the Anderson theorem, so random scattering from defects and impurities should reduce if the elastic mean-free-path is smaller than the superconducting coherence length Mackenzie2003 (). Values of  nm and  nm were observed for YPtBi Butch2011 (); Bay2012 (), but superconductivity was also reported in a case where the mean free path based on free-electron theory, i.e. with is smaller than the lattice constant Shekhar2013 (). This indicates that YPtBi is superconducting even in the dirty limit, which apparently contradicts the hypothesis of -wave superconductivity. A remarkable side-note is that many Half-Heusler compounds are known as semiconductors that show large thermoelectric power at appropriate doping. Even though the carrier concentrations are often high, superconductivity has never been reported for any of these compounds Graf2011 ().

Based on the analysis of the electron-phonon coupling and comparison with experimental data on the normal-state properties it is safe to conclude that an unconventional mechanism is responsible for the superconductivity in YPtBi. Related compounds from the class of topological Half-Heusler semimetals, PtBi and PdBi (with a rare-earth element ) have very similar normal-state properties as YPtBi and also show superconductivity with critical temperatures up to 1.8 K. It is most likely that an unconventional pairing mechanism is at work in all of these compounds. More experimental work, in particular careful studies on the interplay between structural order, normal state electronic properties and superconductivity are necessary to gain more systematic knowledge about the pairing mechanism and the parity of the Cooper pairs. From the theoretical point of view it is particularly challenging to identify pairing mechanisms that allow for sufficiently strong coupling despite the low Fermi density of states, for example an electron-electron coupling assisted by plasmons Takada1980 ().

Acknowledgements.
Calculations leading to the results presented here were performed in part on resources provided by the Paderborn Center for Parallel Computing. The author thanks Thomas Dahm for fruitful discussions.

References

  • (1) H. Lin, L. A. Wray, Y. Xia, S. Xu, S. Jia, R. J. Cava, A. Bansil, and M. Z. Hasan, Nat. Mater. 9, 546 (2010).
  • (2) W. Al-Sawai, H. Lin, R. S. Markiewicz, L. A. Wray, Y. Xia, S. Y. Xu, M. Z. Hasan, and A. Bansil, Phys. Rev. B 82, 125208 (2010).
  • (3) W. Feng, D. Xiao, Y. Zhang, and Y. Yao, Phys. Rev. B 82, 235121 (2010).
  • (4) X.-L. Qi and S.-C. Zhang, Rev. Mod. Phys. 83, 1057 (2011).
  • (5) C. Liu, Y. Lee, T. Kondo, E. D. Mun, M. Caudle, B. N. Harmon, S. L. Budko, P. C. Canfield, and A. Kaminski, Phys. Rev. B 83, 205133 (2011).
  • (6) C. Shekhar, S. Ouardi, A. K. Nayak, G. H. Fecher, W. Schnelle, and C. Felser, Phys. Rev. B 86, 155314 (2012).
  • (7) B. Nowak, O. Pavlosiuk, and D. Kaczorowski, J. Phys. Chem. C 119, 2770 (2015).
  • (8) G. Goll, M. Marz, A. Hamann, T. Tomanic, K. Grube, T. Yoshino, and T. Takabatake, Physica B: Condens. Matt. 403, 1065 (2008).
  • (9) C. Shekhar, M. Nicklas, A. K. Nayak, S. Ouardi, W. Schnelle, G. H. Fecher, C. Felser, and K. Kobayashi, J. Appl. Phys. 113, 17E142 (2013).
  • (10) F. F. Tafti, T. Fujii, A. Juneau-Fecteau, S. Rene de Cotret, N. Doiron-Leyraud, A. Asamitsu, and L. Taillefer, Phys. Rev. B 87, 184504 (2013).
  • (11) G. Xu, W. Wang, X. Zhang, Y. Du, E. Liu, S. Wang, G. Wu, Z. Liu, and X. X. Zhang, Sci. Rep. 4, 5709 (2014).
  • (12) Y. Nakajima, R. Hu, K. Kirshenbaum, A. Hughes, P. Syers, X. Wang, K. Wang, R. Wang, S. R. Saha, D. Pratt, J. W. Lynn, and J. Paglione, Sci. Adv. 1500242 (2015).
  • (13) M. Sigrist, D. F. Agterberg, P. A. Frigeri, N. Hayashi, R. P. Kaur, A. Koga, I. Milat, K. Wakabayashi, and Y. Yanase, J. Magn. Magn. Mater. 310, 536 (2007).
  • (14) M. Sato and S. Fujimoto, Phys. Rev. B 79, 094504 (2009).
  • (15) M. Leijnse and K. Flensberg, Semicond. Sci. Technol. 27, 124003 (2012).
  • (16) R. A. Hein, J. W. Gibson, R. Mazelsky, R. C. Miller, and J. K. Hulm, Phys. Rev. Lett. 12, 320 (1964).
  • (17) P. B. Allen and M. L. Cohen, Phys. Rev. 177, 704 (1969).
  • (18) J. F. Schooley, W. R. Hosler, E. Ambler, J. H. Becker, M. L. Cohen, and C. S. Koonce, Phys. Rev. Lett. 14, 305 (1965).
  • (19) E. Bustarret, Phys. C Supercond. Appl. 514, 36 (2015).
  • (20) Y. Takada, J. Phys. Soc. Japan 49, 1267 (1980).
  • (21) E. A. Ekimov, V. A. Sidorov, E. D. Bauer, N. N. Mel’nik, N. J. Curro, J. D. Thompson, and S. M Stishov, Nature 428, 542 (2004).
  • (22) Y. S. Hor, A. J. Williams, J. G. Checkelsky, P. Roushan, J. Seo, Q. Xu, H. W. Zandbergen, A. Yazdani, N. P. Ong, and R. J. Cava, Phys. Rev. Lett. 104, 057001 (2010).
  • (23) X.-L. Zhang and W.-M. Liu, Sci. Rep. 5, 8964 (2015).
  • (24) S. Das Sarma and Q. Li, Phys. Rev. B 88, 081404 (2013).
  • (25) D. Li, B. Rosenstein, B. Y. Shapiro, and I. Shapiro, Phys. Rev. B 90, 054517 (2014).
  • (26) N. P. Butch, P. Syers, K. Kirshenbaum, A. P. Hope, and J. Paglione, Phys. Rev. B 84, 220504 (2011).
  • (27) T. V. Bay, T. Naka, Y. K. Huang, and A. de Visser, Phys. Rev. B 86, 064515 (2012).
  • (28) T. V. Bay, M. Jackson, C. Paulsen, C. Baines, A. Amato, T. Orvis, M. C. Aronson, Y. K. Huang, and A. de Visser, Solid State Commun. 183, 13 (2014).
  • (29) P. Giannozzi, S. Baroni, N. Bonini, M. Calandra, R. Car, C. Cavazzoni, D. Ceresoli, G. L. Chiarotti, M. Cococcioni, I. Dabo, A. Dal Corso, S. de Gironcoli, S. Fabris, G. Fratesi, R. Gebauer, U. Gerstmann, C. Gougoussis, A. Kokalj, M. Lazzeri, L. Martin-Samos, N. Marzari, F. Mauri, R. Mazzarello, S. Paolini, A. Pasquarello, L. Paulatto, C. Sbraccia, S. Scandolo, G. Sclauzero, A. P. Seitsonen, A. Smogunov, P. Umari, and R. M. Wentzcovitch, J. Phys. Condens. Matter 21, 395502 (2009).
  • (30) A. Dal Corso, Phys. Rev. B 82, 075116 (2010).
  • (31) A. Dal Corso, Comp. Mat. Sci. 95, 337 (2014).
  • (32) http://elk.sourceforge.net
  • (33) M. Wierzbowska, S. de Gironcoli, P. Giannozi, arXiv:cond-mat/0504077v2
  • (34) E. R. Margine and F. Giustino, Phys. Rev. B 87, 024505 (2013).
  • (35) P. B. Allen and R. C. Dynes, Phys. Rev. B 12, 905 (1975)
  • (36) Y. Takada, J. Phys. Chem. Solids 54, 1779 (1993).
  • (37) P. G. Pagliuso, C. Rettori, M. E. Torelli, G. B. Martins, Z. Fisk, J. L. Sarrao, M. F. Hundley, and S. B. Oseroff, Phys. Rev. B 60, 4176 (1999).
  • (38) T. Oguchi, Phys. Rev. B 63, 125115 (2001).
  • (39) A. P. Mackenzie and Y. Maeno, Rev. Mod. Phys. 75, 657 (2003).
  • (40) T. Graf, C. Felser, and S. S. P. Parkin, Prog. Solid State Chem. 39, 1 (2011).
Comments 0
Request Comment
You are adding the first comment!
How to quickly get a good reply:
  • Give credit where it’s due by listing out the positive aspects of a paper before getting into which changes should be made.
  • Be specific in your critique, and provide supporting evidence with appropriate references to substantiate general statements.
  • Your comment should inspire ideas to flow and help the author improves the paper.

The better we are at sharing our knowledge with each other, the faster we move forward.
""
The feedback must be of minimum 40 characters and the title a minimum of 5 characters
   
Add comment
Cancel
Loading ...
169693
This is a comment super asjknd jkasnjk adsnkj
Upvote
Downvote
""
The feedback must be of minumum 40 characters
The feedback must be of minumum 40 characters
Submit
Cancel

You are asking your first question!
How to quickly get a good answer:
  • Keep your question short and to the point
  • Check for grammar or spelling errors.
  • Phrase it like a question
Test
Test description