Abstract
Surfaces of threedimensional topological insulators have emerged as one of the most remarkable states of condensed quantum matter where exotic electronic phases of Dirac particles should arise. Here we report on superconductivity in the topological insulator Sb_{2}Te_{3} with transition to zero resistance induced through a minor tuning of growth chemistry that depletes bulk conduction channels. The depletion shifts Fermi energy towards the Dirac point as witnessed by a factor of 300 reduction of bulk carrier density and by the largest carrier mobility (≳25,000 cm^{2} V^{−1} s^{−1}) found in any topological material. Direct evidence from transport, the unprecedentedly large diamagnetic screening, and the presence of ∼25 meV gaps detected by scanning tunnelling spectroscopy reveal the superconducting condensate to emerge first in surface puddles, with the onset of global phase coherence at ∼9 K. The rich structure of this state lends itself to manipulation via growth conditions and the material parameters such as Fermi velocity and mean free path.
Introduction
Unconventional superconductivity involving electron bands with nontrivial topological character has been predicted^{1,2,3,4,5} to arise on the surfaces of threedimensional topological insulators (TIs), where conduction channels host helical Dirac fermions^{6,7,8,9,10} that cannot be destroyed by nonmagnetic scattering processes. Such topological superconductors are expected to host unusual Majorana modes^{1} with special nonAbelian statistics^{11} and usher in new approaches to quantum device engineering and materials science. The superconducting phases in topological insulators reported thus far, obtained for example, by Cu doping^{12,13,14} or under very high (GPa range) pressures^{15,16}, were found to have increased bulk carrier densities^{12} and thus appear to be of bulk origin.
Here we report that surface superconductivity in the topological material Sb_{2}Te_{3} with holelike (ptype) bulk conduction can be induced at a remarkably high temperature by a very minor change in Te vapour pressure during the crystal growth. Tellurium overpressure makes no detectable structural changes, yet results in a sharply localized and evidently nonmonotonic doping effect^{17,18}: in this process electrons are supplied to the system in a narrow range of Te vapour pressure (in the vicinity of ∼1.4 MPa), reducing free hole density by over two orders of magnitude, as compared with the samples grown at higher or lower vapour pressures. The net effect is an upshift of the Fermi energy from the bulk valence bands towards the vicinity of the Dirac point, with concurrent enhancement of carrier mobility from the typical μ≲200 cm^{2} V^{−1} s^{−1} in the nonsuperconducting samples to the unprecedented value of ≳25,000 cm^{2} V^{−1} s^{−1} in the superconducting phase. The induced nonmonotonically doped state displays a superconducting resistive transition at a relatively high temperature T_{c}∼9 K. However, quite unexpectedly, the onset of enhanced diamagnetic response, as probed both by a.c. susceptometry and by superconducting quantum interference device (SQUID) magnetometry, takes place well above this temperature. Furthermore, scanning tunnelling spectroscopy (STS) indicates a patchy landscape of superconducting regions with gaps in the differential conductance that can be locally as large as ∼25 meV. The dramatic reduction of net density of free and hugely mobile holes in the material’s bulk and electronic surface inhomogeneity, accompanied by large nonLandau fluctuationlike^{19} diamagnetic signal that displays strong field, temperature and frequency dependence, are all pointing to a nontrivial superconducting state. While the 9 K superconductivity at ambient pressure in a topological material with reduced carrier density is unusual in its own right, our observation of enhanced mobility and strong precursor effects at much higher temperatures points to an inchoate superconducting instability of topological surface states. Notwithstanding presently rudimentary undestanding of the connection between high temperature precursors and T_{c} itself, our results raise a possibility of engineering even higher transition temperatures through controlled tuning of charge doping during materials’ growth.
Results
Salient features of superconductivity in Sb_{2}Te_{3}
We begin by highlighting the most prominent features of our discovery. Fig. 1a shows resistivity of Sb_{2}Te_{3} synthesized under ∼1.4 MPa Te vapour pressure during the hightemperature step of the crystal growth cycle (see Methods) and measured at ambient pressure. The system undergoes a transition to zero resistance at the onset temperature T_{c}≅8.6 K. We note that this is the highest transition temperature observed in a topological material at ambient pressure after synthesis (for chemical and structural analysis, and sample statistics see Methods, Supplementary Figs 1 and 2, and Supplementary Table 1). In the narrow Te pressure range 1.2<P<1.5 MPa, where superconductivity is found, the bulk hole density obtained from Hall resistivity is reduced by over two orders of magnitude (Fig. 1b, Supplementary Fig. 3 and Supplementary Table 1) to ≲10^{18} cm^{−3}—a finding which should be contrasted with the increased electron density recorded in, for example, superconducting Bi_{2}Se_{3} doped with Cu (ref. 12).
In the same narrow pressure range the diamagnetism is enhanced by two orders of magnitude (Fig. 1b) relative to the signal in samples outside the critical pressure range^{20}. STS (Fig. 1c–e, also Methods, Supplementary Fig. 4 and Supplementary Note 1) shows very flat hexagonally ordered surfaces and a clear presence of gaps in differential conductance dI/dV with clear coherence peaks (Fig. 1e) as well as more complex gap structures that can vary locally from 0 to ≳20 meV. This patchy gap landscape indicates a laterally inhomogeneous superconducting state which within BCS theory (using the BCS gap equation 2Δ(0)=3.5k_{B}T_{c}, where k_{B} is the Boltzmann constant) has local transition temperatures that can be as high as 60 K, that is, much greater than the observed resistive T_{c}, but inline with the temperature at which the onset of the enhanced diamagnetic signal is observed discussed below.
Magnetic fieldtemperature phase diagram
Next we turn to the finite field response of the superconducting state. The resistive transition downshifts and broadens with increasing external magnetic field (Fig. 2a,b). By tracking onset temperature T_{c}(H) we map the fieldtemperature H–T phase diagram for the two field orientations: applied along the c axis of the crystal, H  c, and parallel to the ab plane, H  ab (Fig. 2a,b, respectively). The lowtemperature anisotropy of the field H_{R}(T) shown in Fig. 2c (obtained from the resistive onset marked by arrows in Fig. 2a) at first glance is surprisingly small, only ∼1.4, given the large structural anisotropy of Sb_{2}Te_{3} (Supplementary Figs 1 and 2). This anisotropy corresponds nearly exactly to the anisotropy of the gfactor detected by microwave spectroscopy^{21}, , an observation consistent with the limiting field being largely governed by spin rather than orbital effects. If indeed depairing is of paramagnetic (Zeeman) origin, a simple relationship between the paramagnetic field (so called, Chandrasekhar–Clogston limit), H_{p}, and the superconducting transition temperature T_{c} is conventionally obtained^{22} by comparing magnetic energy with the superconducting condensation energy . Here N(0) is the density of states at the Fermi energy, g is the Landé gfactor and Δ(0) and H_{p}(0) are zerotemperature superconducting gap and paramagnetic limiting field, respectively. Equating the observed low temperature values of H_{R}∼3–4 T with H_{P}(0) and using large g values of ≅50 obtained in experiments^{23}, we get an estimate of ∼60 K, which is substantially higher than T_{c}∼9 K but remarkably consistent with the scales of scanning tunnelling microscopy (STM) gap values.
Given this surprising disparity between the observed T_{c}=8.6 K and temperature scale deduced from limiting field (and STM gaps) it is only natural to consider the possibility of inhomogeneous superconducting state in Sb_{2}Te_{3}, with locally superconducting and normalmetal regions coexisting above and somewhat below the resistive transition. Another strong indication of the inhomogeneity comes in the appearance of pronounced de Haas–van Aphen (dHvA) quantum oscillations of magnetization in the superconductng state (inset in Fig. 2c and Fig. 3a,b). The amplitude of dHvA signal in our superconducting Sb_{2}Te_{3} changes rather uneventfully across H_{R}(T) and shows no additional damping below the limiting field (Supplementary Fig. 5). This is quite unlike a more conventional behaviour in uniform type II superconductors^{24}, where dHvA oscillations are strongly damped at fields lower than the upper critical field, H_{c2}.
de Haas van Alphen oscillations and 2DEG
Quantum dHvA oscillations are one of the most direct probes of quasiparticle excitations in metals^{25}, and in superconducting Sb_{2}Te_{3} are quite remarkable in their own right as they clearly display a beat structure (Figs 2c and 3a–c, Supplementary Figs 5 and 6 and Supplementary Note 2) similar to that found in spinorbit coupled quantum well states in semiconductors^{26}. Lifshitz–Kosevich analysis^{25} of these oscillations (Supplementary Fig. 5 and Supplementary Table 2) yields v_{F}≃5.3 × 10^{5} ms^{−1}, ℓ≈95 nm, m=0.065 m_{e}, k_{F+}=3.7 × 10^{8} m^{−1}, k_{F−}=3.3 × 10^{8} m^{−1} for Fermi velocity, meanfree path, effective mass and the two close Fermi wave vectors that induce the beats, respectively. The overall beat structure appears to scale with the magnetic field component transverse to the surface as shown in Fig. 3c for three field orientations, suggestive of the twodimensional (2D) character of the beat signal. Nontopological but largely 2D bulklike states have been predicted in TIs in ab initio calculations^{27} and detected in angleresolved photoemission spectroscopy^{28} but, to the best of our knowledge, have never been observed in magnetooscillations—our observation may be the first such detection of such (sub)surface excitations. The peculiar dispersion of the bulk valence bands^{7} of Sb_{2}Te_{3} suggests the mechanism by which Te overpressure promotes the visibility of 2D electron gas (2DEG; Fig. 3d)—in the narrow region of Te overpressure the hole density is severely reduced, bringing the Fermi level up to just below the Dirac point where it intersects the surface state and six small pockets of bulk bands which are expected to participate in band bending and surface reconstruction of electronic structure.
Huge carrier mobility consistent with surface transport
Carrier mobility can be estimated from either transport data or Dingle analysis^{25} of the dHvA data. A priori, these two methods need not agree and in the nonsuperconducting TIs, including Sb_{2}Te_{3} (see Supplementary Table 2), this is the case; in transport the usual Drude description of conductivity mixes all participating bulk and surface channels (particularly when there are multiple pockets in the Brillouin zone) while dHdA is sensitive mostly to the highest mobility paths. Remarkably, in superconducting samples, we obtain very similar values of 25,000 cm^{2} V^{−1} s^{−1} and 26,600 cm^{2} V^{−1} s^{−1} from transport and dHvA, respectively, roughly within the experimental uncertainty (Supplementary Table 2). These values are exceptionally high compared to our nonsuperconducting samples (where mobility is a factor of ∼165 smaller and mean free path ℓ is a factor of four smaller,Supplementary Table 2), but also to the values in other TIs^{29,30,31}. The consistency of both estimates and the appearance of hugely mobile holes in the superconducting state suggest that here mostly surface conducting channels are involved.
Unusual hightemperature diamagnetic response
Now, we return to examine the diamagnetic signal shown in Fig. 1b. Differential diamagnetic magnetic susceptibility (Fig. 4a–c) measured using a relatively low (10 kHz) frequency is strongly field and temperature dependent. The signal persists to high temperatures as it smoothly and monotonically reduces to nonsuperconducting values. This unusual differential response is found to vary strongly with frequency of a.c. excitation even for the low (∼kHz) frequencies used (Fig. 4d,e). Conventional bulk superconductors do not exhibit such frequency dependence, however, inhomogeneous superconductors often do^{32,33} and therefore require a considerably more comprehensive and nuanced approach to reliably relate magnetic signatures to superconductivity, which we now present.
General analyticity considerations at low external field dictate that low frequency dependence is analytic and can be approximated quadratically, , and such behaviour is found in resistively shunted Josephson networks and other cases of two fluid (normal+superfluid) dynamics^{32}. With this in mind we analysed the frequency dependence of by performing frequency scans at different temperatures, focusing on the low field regime. The data (inset in Fig. 4g) clearly follows a parabolic frequency dependence. The fit to this simple form uncovers a spectacular dichotomy between temperature variation of the zero frequency value (Fig. 4g, Supplementary Note 3 and Supplementary Fig. 7) and the dispersion coefficient b(T) (Fig. 4f): shows a sharp diamagnetic onset in the vicinity of ∼55 K, while the prefactor b(T) smoothly marches toward the near null value at very high temperatures (see also Supplementary Fig. 7 and Supplementary Note 4). For completeness, we also examined the imaginary part of magnetic susceptibility and it clearly exhibits conventional eddy current heating behaviour (Supplementary Fig. 8).
Mesoscopic superconducting puddles in Sb_{2}Te_{3}
This sharp variation of is closely mirrored both in its saturation magnitude, ∼10^{−4} e.m.u. cm^{−3} (Fig. 4g), and in the onset temperature of 55 K in d.c. magnetization measured using SQUID (Fig. 4h). The absolute value of diamagnetic response obtained in these samples clearly exceeds those of typical topological insulators (and semiconductors generally) by at least two orders of magnitude^{20,34} but also the largest known diamagnetic susceptibilities of semimetals^{35,36,37}. Thus, we identify the pronounced variation (with temperature, field and/or frequency) and the overall magnitude of the diamagnetic response with a mesoscopic Meissner transition near 50 K detected in SQUID (Fig. 4g). We observe that the finite frequency response coefficient, b(T), varies smoothly and persists to much higher temperatures (see Fig. 4f), well above 100 K—this indicates a distribution of superconducting regions (puddles). Significantly, both and b in relatively thick (∼mm size) samples exhibit a large field anisotropy (Fig. 4f) consistent with the 2D nature of diamagnetic response and with the surface origin of the signal. Notably, the mesoscopic diamagnetic transition near 50–55 K is also mirrored in transport, whereby resistivity exhibits a clear downward step that broadens and disappears in finite fields, consistent with the existence of finitesized superconducting shorts inside the sample (Supplementary Fig. 9).
Discussion
There are three most noteworthy aspects of the new electronic state in Sb_{2}Te_{3}. One is the uncovered extreme sensitivity to the growth parameters that reveals an instability to strong correlations, leading to our discovery of superconductivity at ambient pressure and relatively high temperature of ∼8.6 K. It illuminates a path to topological superconductivity by finetuned doping control. Another is its likely surface origin as seen through the unexpectedly suppressed bulk charge carrier density, ordersofmagnitude enhanced carrier mobility and extreme anisotropy of diamagnetic screening. And the third is a clear evidence of mesoscopic either remnants or precursors persisting to much higher temperatures, detected by four kinds of independent probes employed in our studies, namely, transport, a.c. susceptibility, d.c. magnetization, and STM and witnessed by a distinct (low) frequency response.
Resemblant precursor effects are well established in systems where superconducting grains are imbedded in a metallic or insulating matrix^{38,39,40}. It should be noted that puddles have been known to form at low carrier densities in other 2D Dirac systems^{41} owing to nonlinear screening effects^{42,43} and surface Dirac puddles have been reported in STS studies of doped nonsuperconducting TIs^{44}. So it is natural to ask what additional insights might be attained if we consider the existence of similar mesoscopic structures imbedded in the high mobility metallic matrix apparent from our dHvA results.
To start then, we expect that the observed resistive transition is due to percolation of proximity induced couplings, that is, it is not of BCS meanfield character and should exhibit different (stronger) fluctuation effects^{19}. Well below the resistive transition the mesoscopic character of the state is lost due to proliferation of such proximity couplings, that is, the gap function is expected to decay very slowly inside the metallic matrix. Our low temperature STM scans have uncovered inhomogeneity in the gap function on very long scales, larger than available sampling density of regions (Supplementary Fig. 4), which is fully consistent with the dominance of proximity coupling for T<T_{c}≈9 K. The percolative model of the transition^{38,45} allows us to obtain rough estimates of interpuddle spacing a and puddle size R, which we now summarize (a more detailed discussion is in Supplementary Notes 4 and 5). The typical interpuddle distance must be comparable to the diffusive length L_{T} of the metallic matrix at T_{c}, a≈L_{T}. We estimate L_{T} from the dHvA data to be ≈140 nm. Assuming that all puddles reside on the surface allows us to estimate the total number of puddles in the sample (≲10^{9}) and, furthermore, the typical puddle’s lateral size, R≈37 nm, from the observed magnetization signal at low fields directed along the c axis. This phenomenological analysis consistently and quantitatively connects all of the low temperature experimental observations, including the resistive transition, its inhomogeneous and nearly isotropic suppression in strong fields, strong anisotropy of the diamagnetic screening, and STM maps.
Local superconductivity on mesoscopic scales in the globally normal state should be detectable as fluctuationlike phenomena in resistivity and other probes, including magnetization. At the simplest (mean field) level we expect that for a single superconducting puddle smaller than penetration depth, , in the otherwise normal metal to contribute to the diamagnetic susceptibility^{46} and a downward step^{22} in resistivity R(T). Magnetization data (Fig. 4g,h) and transport (Supplementary Fig. 9) appear to consistently support the existence of an intrapuddle meanfield transition near T≈50 K, which is both much higher than T_{c} but also relatively sharp, hinting at the monodispersity of puddle distribution. Observation of such high temperature scale for the local mesoscopic transition is unprecedented in this or any other semiconductors.
Although several of our experimental findings can be consistently understood in the phenomenological framework of superconductormetal composite system, the nature of the putative superconductivity in the puddles remains to be elucidated. For one, the weak anisotropy of the resistive limiting field implies that spin physics and spinorbit coupling play a significant role in establishing the resistive H versus T phase diagram via paramagnetic depairing mechanism^{22}. Also mesoscopic fluctuations in the effective Josephson network governing the resistive transition^{45} must play a role in the observed variations in transport and in significant superconducting fluctuations at high temperatures. We remark that 2D superconductivity that has been found in 2DEG at the interfaces between two band insulators, LaAlO_{3} and SrTiO_{3} occurs below 200 mK (ref. 47), a much lower temperature than we observe; the much higher T_{c} in Sb_{2}Te_{3} is a likely spillover from the superconducting puddles^{48} supporting pairing of helical Dirac holes.
Methods
Crystal growth
Single crystals of Sb_{2}Te_{3} were grown in evacuated quartz tubes in a horizontal gradient furnace heated to 1,000 °C and cooled to room temperature in 7–10 days. The starting materials used were cmsized chunks of Sb (purity 99.9999%) and Te (purity 99.9995%) from Alfa Aesar used in stoichiometric ratios. We made over 20 crystal growth runs under similar growth conditions and screened all samples, usually approximately millimetre in size, for their overall diamagnetic response using a.c. susceptibility first. The critical parameter was Te pressure during the high temperature segment of the growth process; it was determined from the ideal gas equation P=nRT_{max}/V, where T_{max} is the highest temperature used, V is the enclosed volume, n is the umber of moles of the material and R is the ideal gas constant; it was consistent with equilibrium binary phase diagram of Sb–Te (ref. 49).
Chemistry of crystal growth from the stoichiometric melt in a fixed volume at high (1,000 °C) temperature sets the stoichiometry of the final crystal product. To finetune Te pressure for each crystal growth run we were changing the sealed tube volume while keeping the starting materials in stoichiometric ratio and the melt temperature fixed. The key physical consequence of Te overpressure in the 1.2–1.5 MPa pressure range was the reduced hole density and enhanced mobility. Since the topographic and structural integrity and robustness of crystalline surfaces are unaltered, these huge changes in transport give us important information regarding the contribution of surface conduction channels relative to the bulk. In the bulk there are charge carriers donated by intrinsic crystalline lattice defects, such as vacancies and antisites. In Sb_{2}Te_{3} vacancies on cation (Sb) or anion (Te) sites respectively act as electron donors and acceptors. From the detailed studies of these materials^{17,50} we know that growth conditions using stoichiometric ratio starting materials result in slightly Te poor crystals, Sb_{2}Te_{3–x} with x≈0.03–0.05. Also, native concentrations of Sb antisites (contributing one hole each) and Te vacancies (contributing two electrons each) are ∼10^{20} cm^{−3} and 2 × 10^{19}cm^{−3}, respectively, consistently accounting for the observed Hall number and other material properties^{17,18}. As Te pressure during the growth is increased, a fully stoichiometric (2:3) crystalline material is obtained in which bulk carrier density is the lowest. Under the growth conditions with Te pressure exceeding ∼1.5 MPa, the process is reversed since as the system becomes slightly Te rich (or Sb poor), the antisite defects delivering holes to the bulk are less likely to form and the hole density is increased again. This change in stoichiometry is very slight and transport is the best way to detect it. We note that such finetuned nonmonotonic doping is not unprecedented; it has been also observed in Sb_{2}Te_{3} doped with Cr (ref. 17), in molecularbeam grown epitaxial TI films^{51}, and upon stoichiometry variation in Bi–Sb–Te system grown by zone melting^{52}.
Structural characterization and elemental analysis
The structure and composition of crystals grown in the 0.4–3 MPa pressure range was determined from Xray diffraction and glow discharge analysis (Evans Analytical Group) that determined impurity content (< 0.6 p.p.m. wt) of the final crystals (Supplementary Table 1). Xray diffraction (Supplementary Fig. 1a) was performed in Panalytical diffractometer using Cu line from Philips high intensity ceramic sealed tube (3 kW) Xray source with a Soller slit (0.04 rad) incident and diffracted beam optics. Structural identity was confirmed by microRaman spectroscopy of characteristic phonon modes (Supplementary Fig. 1b).
Scanning tunneling spectroscopy measurements
STM and STS measurements were carried out in a homebuilt cryogenic UHV STM at a temperature of 4.8 K (Supplementary Fig. 4 and Supplementary Note 1). STM studies were performed on five samples. Spectroscopy measurements were performed using a lockin amplifier running at a frequency of 1.831 kHz and an excitation voltage of 0.2 mV. Spectroscopic imaging was carried out on five samples over a grid of points (either 128 × 128 or 256 × 256 pixels) at various energies using the same lockin amplifier parameters. Fourier transforms are affine transformed to correct for drift and then hexagonally averaged to enhance signal to noise.
Transport and susceptibility measurements
Transport and susceptibility measurements were performed in a 14 T Quantum Design PPMS system in 1 mT of He gas. For transport measurements, lithographically patterned Au/Ti contacts in Hall bar and van der Pauw geometries were fabricated on 100–300nm thin crystals exfoliated onto SiO_{2}/Si substrates. The typical uncertainty in transport measurements was ∼0.1%. Out of seven samples three exhibited zero field resistive transition with T_{c}∼9 K. Two were used for mapping the H versus T phase diagram in Fig. 2, two were used for a careful measurement of the high temperature resistive feature near 50 K. Carrier densities were determined from Hall resistivity and dHdA oscillations (Supplementary Table 2). Differential susceptibility was measured in a compensated pickupcoil detection configuration with the excitation/detection coils designed to align with the applied static field^{20}. The measurement uncertainty was <1%. The a.c. excitation amplitude was set at 10^{−5} T in a frequency range up to 10 kHz. The system was calibrated using paramagnetic Pd standard and superconducting Nb. Susceptibility calibration and measurements of small background contribution are described in ref. 20. d.c. magnetization measurements were performed using Quantum Design SQUID Magnetometer in up to 5.5 T fields. In all magnetic measurements the samples were supported in gelcaps without any substrates. The uncovered huge diamagnetic enhancement for the samples grown in the 1.4–1.5 MPa range was 100% robust and reproducible.
Additional information
How to cite this article: Zhao, L. et al. Emergent surface superconductivity in the topological insulator Sb_{2}Te_{3}. Nat. Commun. 6:8279 doi: 10.1038/ncomms9279 (2015).
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Acknowledgements
We are grateful to David Huse, Steven Kivelson, Boris Spivak, Kyungwha Park, Kamran Behnia, Steven Girvin, Shivaji Sondhi and Alexander Gurevich for enlightening discussions. V.O. wishes to acknowledge stimulating discussions with Jeremy Levy and Sarang Gopalakrishnan. We thank Jeff Secor for the technical assistance with Raman spectroscopy. This work was supported in part by NSF under DMR1122594 (L.K.E.), DMR1420634 (A.P., L.K.E. and V.O.), DMR1322483 (L.K.E.), DMR0955714 (V.O.), and by DODW911NF1310159 (L.K.E.).
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Experiments were designed by L.K.E. and L.Z. L.Z. and H.D. carried out the growth of the single crystals, I.K. and Z.C. provided structural and chemical characterization, and H.D, L.Z. and M.B. designed and fabricated exfoliated structures with lithographic contacts. Transport and magnetic measurements were performed by L.Z. and H.D., STS and STM experiments were performed by E.A., E.R. and A.P., and data analysis was done by L.Z., V.O. and L.K.E. All authors discussed the results, and V.O., L.Z. and L.K.E. contributed to the writing of the manuscript.
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Supplementary Figures 19, Supplementary Tables 12, Supplementary Notes 15 and Supplementary References (PDF 1369 kb)
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Zhao, L., Deng, H., Korzhovska, I. et al. Emergent surface superconductivity in the topological insulator Sb_{2}Te_{3}. Nat Commun 6, 8279 (2015). https://doi.org/10.1038/ncomms9279
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DOI: https://doi.org/10.1038/ncomms9279
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