Gate-induced superconductivity in a monolayer topological insulator

See allHide authors and affiliations

Science  23 Nov 2018:
Vol. 362, Issue 6417, pp. 922-925
DOI: 10.1126/science.aar4426

A monolayer of many talents

Superconductors with a topologically nontrivial band structure have been predicted to exhibit exotic properties. However, such materials are few and far between. Now, two groups show that the monolayer of the material tungsten ditelluride (WTe2)—already known to be a two-dimensional topological insulator—can also go superconducting. Fatemi et al. and Sajadi et al. varied the carrier density in the monolayer by applying a gate voltage and observed a transition from a topological to a superconducting phase. The findings may lead to the fabrication of devices in which local gating enables topological and superconducting phases to exist in the same material.

Science, this issue p. 926, p. 922


The layered semimetal tungsten ditelluride (WTe2) has recently been found to be a two-dimensional topological insulator (2D TI) when thinned down to a single monolayer, with conducting helical edge channels. We found that intrinsic superconductivity can be induced in this monolayer 2D TI by mild electrostatic doping at temperatures below 1 kelvin. The 2D TI–superconductor transition can be driven by applying a small gate voltage. This discovery offers possibilities for gate-controlled devices combining superconductivity and nontrivial topological properties, and could provide a basis for quantum information schemes based on topological protection.

Many of the most important phenomena in condensed matter emerge from the quantum mechanics of electrons in a lattice. The periodic potential of the lattice gives rise to Bloch energy bands of independent fermions; on the more exotic side, electrons in a lattice can pair up into bosons and condense into a superconducting macroscopic quantum state, which conducts electricity with zero resistance. Relatively recently, it was realized that Bloch wave functions can have a nontrivial topology, leading to the discovery of topological insulators—materials that are electrically insulating in their interior but have conducting boundary modes (1). The first of these to be studied was the so-called 2D topological insulator (2D TI), in which 1D helical edge modes (spin locked to momentum) give rise to the quantum spin Hall effect (24).

Materials that combine nontrivial topology with superconductivity have been the subject of active investigation in recent years (57). Here, we report that monolayer WTe2, recently shown (813) to be an intrinsic 2D TI, turns superconducting under moderate electrostatic gating. Several other nontopological layered materials superconduct in the monolayer limit, either intrinsically or under heavy doping using ionic liquid gates (1422). In monolayer WTe2, however, the phase transition to a superconducting state is from a 2D topological insulator, and it occurs at such a low carrier density that it can be readily induced by a simple electrostatic gate. The discovery may lead to gateable superconducting circuitry and may enable the development of topological superconducting devices in a single material, as opposed to the hybrid constructions currently required (5).

We present data from two monolayer WTe2 devices, M1 and M2, with consistent superconducting characteristics. Each contains a monolayer flake of WTe2 encapsulated along with thin platinum electrical contacts between hexagonal boron nitride (hBN) dielectric layers. Figure 1A shows an image of M1, which has seven contacts along one edge, together with a side view and a schematic showing the configuration used to measure the linear four-probe resistance, Rxx = dV/dI. Top and bottom gates—at voltages Vt and Vb and with areal capacitances ct and cb, respectively—can be used to induce negative or positive charge in the monolayer WTe2, producing an areal doping density given by ne = (ctVt + cbVb)/e, where e is the electron charge. Note that we do not interpret this as a carrier density because the insulating state may be of correlated nature (as in, for example, an excitonic insulator); in addition, Hall density measurements are challenging because of the 2D TI edge conduction. See (23) for details about gating, contact resistances, and capacitances.

Fig. 1 Characteristics of monolayer WTe2 device M1 at temperatures below 1 K.

(A) Optical image (scale bar, 5 μm) of M1 and schematic device structure of a sample with two graphite gates, showing current, voltage contacts, and ground configuration for measuring the four-probe resistance Rxx. Inset: Schematic of the atomic structure of monolayer WTe2. (B) Rxx as a function of electrostatic doping (ne) at a series of temperatures. Inset: Variation of Rxx at 20 mK with top and bottom gate voltages, Vt and Vb, indicating the axes corresponding to doping ne and transverse displacement field D. Rxx depends primarily on ne and only weakly on D. The measurements in the main panel for ne > 0 and ne < 0 were made separately, sweeping Vb along the two colored dashed lines in the inset to avoid contact effects. (C) Phase diagram constructed from measurements in this paper.

Figure 1B illustrates the electrostatic tuning of M1 from p-doped conducting behavior at negative gate voltage, through an insulating state, to an n-doped highly conducting state at positive gate voltage. M1 is the same device whose insulating state was investigated in (9) and was demonstrated to be a 2D TI (9, 13); at ne = 0, Rxx is more than 107 ohms, owing to a meV-scale gap that blocks edge conduction below 1 K [see below and (23)]. For ne above ncrit ≈ +5 × 1012 cm–2, however, the resistance drops drastically when the sample is cooled, reaching the noise floor of the experiment (~0.3 ohms) for ne > +7 × 1012 cm–2 at 20 mK, indicating the appearance of superconductivity. Figure 1C is a phase diagram constructed from these and similar measurements discussed below. The emergence of a superconducting phase in direct proximity to a 2D TI phase, and at a doping level achievable with a single electrostatic gate, is the primary result of our work.

The transition from an insulating to a metallic/superconducting T dependence—the crossing of Rxx lines in Fig. 1B—occurs at 2.4 kilohms. This corresponds to a square resistivity ρ ≈ 20 kilohms, with a substantial uncertainty because the precise distribution of current in the device is not known (23). The evolution of the T dependence with ne is illustrated in Fig. 2A. For all densities shown, the collapse of Rxx with temperature is gradual, as expected for materials where the normal-state 2D conductivity is not much greater than e2/h (where h is the Planck constant). We define a characteristic temperature, T1/2, at which Rxx falls to half of its 1 K value. Although this specific definition is somewhat arbitrary, it is typical in the literature (15, 21, 22) and does not affect any of our conclusions (23). Measured values of T1/2 are shown as red dots on the phase diagram in Fig. 1C to indicate the boundary of superconducting behavior.

Fig. 2 Resistance characterization of device M1 in the superconducting regime.

(A) Rxx on log scale versus temperature T at a series of positive-gate doping levels ne [20, 12, 8.5, 6.7, 6.1, 5.6, 5, and 4.6 × 1012 cm–2] showing a drop of several orders of magnitude at low T for larger ne. Inset: Location of sweeps on the phase diagram. (B) Effect of perpendicular magnetic field B on resistance at the highest ne value in (A). (Demagnetization effects are neglected in light of the finite resistivity of the sample.) Inset: Characteristic temperatures T1/2 obtained from these temperature sweeps, as well as characteristic fields B1/2 measured from field sweeps under similar conditions. (C) Same as (B) but for the in-plane magnetic field B|| (the B|| = 0 data are for ne = 19 × 1012 cm–2; the remaining data are for ne = 18 × 1012 cm–2). Inset: Reduction of T1/2 with B||, fit to the expected form for materials with strong spin-orbit scattering (solid line). The Pauli limit BP, assuming g = 2, is indicated by the dashed line. (D) Data from (B) replotted to highlight the saturation of Rxx at low T. (E) Sweeps of B showing rise of resistance beginning at very low field. (F) Sweep of B|| showing sharper onset of resistance relative to (E). Inset: Data from (C) on a linear scale.

The superconductivity is suppressed by a perpendicular (B) or in-plane (B||) magnetic field (Fig. 2, B and C). For a perpendicular field, orbital effects are expected to dominate (2426). The dependence of T1/2 on B (Fig. 2B, inset) in the low-field limit is consistent with the linear Embedded Image expected from Ginzburg-Landau theory. The characteristic perpendicular field in the low-temperature limit, based on the measurements in Fig. 2B (inset), is Embedded Image, where Embedded Image is the magnetic field where Rxx falls to half its normal-state resistance. Estimates for the superconducting coherence length can be obtained either from the slope of Embedded Image near T1/2 or from Embedded Image, yielding ξmeas = 100 ± 30 nm in both cases (23).

The fact that ξmeas is much larger than the estimated mean free path Embedded Image ≈ 8 nm suggests that the system is in the dirty limit (λ << ξ). To calculate λ, we use spin and valley degeneracies gs = gv = 2, as well as density and normal-state resistivity reflecting the conditions for Fig. 2B: ne = 20 × 1012 cm–2 and ρ ≈ 2 kilohms, respectively. The coherence length expected in the dirty limit is Embedded Image, for zero-temperature gap Δ0 = 1.76kBTc and diffusion constant D, where ħ is the reduced Planck constant and kB is the Boltzmann constant. Indeed, if we use T1/2 = 700 mK for Tc, and if D = 2πħ2/gsgvm*e2ρ ≈ 12 cm2 s–1 (from the Einstein relation) with effective mass m* = 0.3me [where me is the electron mass (27)], the result is ξ ≈ 90 nm, consistent with ξmeas.

For the in-plane magnetic field, the atomic thinness of the monolayer makes orbital effects small. In the absence of spin scattering, superconductivity is then suppressed when the energy associated with Pauli paramagnetism in the normal state overcomes the superconducting condensation energy. This is referred to as the Pauli (Chandrasekar-Clogston) limit (28) and gives a critical field BP = 1.76kBTc/g1/2μB, where μB is the Bohr magneton. Assuming an electron g-factor of g = 2 and taking Tc = 700 mK gives BP ≈ 1.3 T. However, the data in Fig. 2, C and F, indicate superconductivity persisting to Embedded Image.

Similar examples of Embedded Image exceeding BP have recently been reported in other monolayer dichalcogenides, MoS2 and NbSe2, but the Ising superconductivity mechanism (15, 21) invoked in those works cannot explain an enhancement of Embedded Image here because WTe2 lacks the required in-plane mirror symmetry. One possible explanation in this case is a high spin-orbit scattering rate Embedded Image. Fitting the predicted form for Tc in a parallel field (29) to the data in the inset of Fig. 2C gives Embedded Image (23). Another possibility is that the Pauli limit is not actually exceeded but that the effective g-factor in WTe2 is smaller than 2 owing to the strong spin-orbit coupling.

The data in Fig. 2 display several other features worthy of mention. First, at intermediate magnetic fields, the resistance approaches a T-independent level as T → 0 that is orders of magnitude below the normal-state resistance. The data from Fig. 2B are replotted versus 1/T in Fig. 2D to highlight the behavior below 100 mK. Similar behavior is seen at B = 0 (Fig. 2A) for intermediate ne, adding to the growing body of evidence that this is a robust phenomenon occurring in thin films close to superconductivity (30). Second, even at the lowest temperature, Rxx rises smoothly from zero as a function of B (Fig. 2E), whereas the onset of measurable resistance as a function of B|| is relatively sudden, occurring above 2 T (Fig. 2F). Third, an intermediate plateau is visible in the RxxT data at B = 0 over a wide range of ne (Fig. 2A). It is extremely sensitive to B, almost disappearing at only 2 mT (Fig. 2B), whereas it survives in B|| to above 2 T (Fig. 2C and inset of Fig. 2F). A similar feature has been reported in some other quasi-2D superconductors (3133), but its nature, and the role of disorder, remain unresolved.

The high tunability of this 2D superconducting system invites comparison with theoretical predictions for critical behavior close to a quantum phase transition. Figure 3 shows how Rxx depends on doping at a series of temperatures, along the dashed lines in the phase diagram (upper inset). The T dependence changes sign at ncrit ≈ 5 × 1012 cm–2. In the lower inset, we show an attempt to collapse the data onto a single function of |1 – ne/ncrit|T–α. The procedure is somewhat hindered by the fluctuations, which can be seen to be largely reproducible. The best-fit critical exponent α = 0.8 is similar to that reported for some insulator-superconductor transitions in thin films (34), although we note that the anomalous behavior near ncrit mentioned above is not consistent with such a scaling.

Fig. 3 Scaling analysis of the transition.

Main panel: Multiple Rxx versus doping traces, taken at different temperatures, cross at a critical doping level ncrit ≈ 5 × 1012 cm–2. Upper inset: Dashed lines locate these sweeps on the phase diagram. Lower inset: The same data presented on a scaling plot, taking critical exponent α = 0.8.

Superconductivity induced by simple electrostatic gating in a monolayer of material that is not normally superconducting is intriguing, but perhaps even more interesting is that the ungated state is a 2D TI. This prompts the question of whether the helical edge channels remain when the superconductivity appears, and if so, how strongly they couple to it. In principle, Rxx includes contributions from edges as well as bulk. However, because in device M1 the edge conduction freezes out below 1 K, in order to investigate the combination of edge channels and superconductivity we turn to another device, M2, in which edge conduction persists to lower temperatures (23).

Figure 4 shows measurements of the conductance G between adjacent contacts in M2 as a function of gate doping. The figure includes schematics indicating the inferred state of the edge (red for conducting), as well as the bulk state (colored to match the phase diagram). Consider first the black trace, taken at 200 mK and B = 0. At low ne, the bulk is insulating and edge conduction dominates, albeit with large mesoscopic fluctuations. For ne > 2 × 1012 cm–2, G increases as bulk conduction begins; then, once ne exceeds ncrit, it increases faster as superconductivity appears, before leveling out at ~200 μS as a result of contact resistance. This interpretation is supported by warming to 1 K (red dotted trace), which destroys the superconductivity and so reduces G for ne > ncrit, but enhances the edge conduction at low ne toward the ideal value of e2/h = 39 μS. (We note that this T dependence of the edge is associated with a gap of ~100 μeV, visible in the inset map of differential conductance versus bias and doping.) A perpendicular field B of 50 mT (green trace) also destroys the superconductivity, causing the conductance to fall for ne > ncrit but barely affecting it at lower ne. High magnetic fields have been shown (9) to suppress edge conduction in the 2D TI state by breaking time-reversal symmetry. This effect can be clearly seen in the B = 1 T data (orange trace in Fig. 4) as G falls to zero at low ne. Comparison of the green (B = 0.05 T) and orange (B = 1T) traces shows that G falls by a similar amount at higher ne, consistent with a scenario in which the edge conduction supplies a parallel contribution; this implies that helical edge states persist when ne > ncrit and at temperatures below Tc.

Fig. 4 Evidence for the presence of both edge conduction and superconductivity in device M2.

The main panel shows the linear conductance between two adjacent contacts versus gate doping at the temperatures and perpendicular magnetic fields noted. Schematics indicate the state of edge and bulk conduction at different points; the bulk is colored to match the phase diagram reproduced above, and red indicates a conducting edge state. Superconductivity occurs for ne > 5 × 1012 cm–2 at B = 0. The zero-resistance state, disguised by contact resistance in this figure, was confirmed in a separate four-wire measurement of R versus T (fig. S10); edge conduction dominates for ne < 2 × 1012 cm–2 but appears to be present at all values of ne. Inset: Color-scale plot of differential conductance versus dc voltage bias and doping level, revealing a gap of ~100 μeV that fluctuates rapidly as a function of doping level.

This discovery raises compelling questions for future investigation. It is likely that the helical edge modes persist when the superconductivity is restored by reducing the magnetic field to zero. Other techniques, such as scanning probe microscopy, may be needed to probe the edges separately from the bulk. The measurements presented here cannot determine the degree or nature of the coupling between superconductivity and edge conduction. One key question is whether the edge states also develop a superconducting gap, in which case they could host Majorana zero modes (5).

Another question concerns the nature of the superconducting order. It is striking that ncrit corresponds to only ~0.5% of an electron per W atom, which is about an order of magnitude lower than the doping level needed to observe superconductivity in other transition metal dichalcogenide monolayers (18). Many-layer WTe2 is semimetallic (3538) under ambient conditions, with near-perfect compensation of electrons and holes, but becomes superconducting as the ratio of electrons to holes increases at high pressure (39). Some related materials, such as TiSe2, are known to switch from charge-density-wave to superconducting states at quite low doping (40) or under pressure (41). We therefore speculate that doping tips the balance in monolayer WTe2 in favor of superconductivity, away from a competing insulating electronic ordering. Finally, given the topological band structure and likely strong correlations in this material, it is possible that the pairing is unconventional and perhaps topologically nontrivial.

Supplementary Materials

Materials and Methods

Supplementary Text

Figs. S1 to S10

Table S1

References (42, 43)

References and Notes

  1. See supplementary materials.
Acknowledgments: We thank O. Agam, A. Andreev, and B. Spivak for discussions, and J. Yan for the WTe2 crystals. Funding: T.P., Y.F., W.Z., X.X., and D.H.C. were supported by the U.S. Department of Energy, Office of Basic Energy Sciences, Division of Materials Sciences and Engineering, awards DE-SC0002197 (D.H.C.) and DE-SC0018171 (X.X.); AFOSR FA9550-14-1-0277; NSF EFRI 2DARE 1433496; and NSF MRSEC 1719797. E.S., P.B., C.O., S.L., and J.A.F. were supported by the Canada Foundation for Innovation, the National Science and Engineering Research Council, CIFAR, and SBQMI. Author contributions: T.P., X.X., and D.H.C. conceived of the original experiment; T.P., Z.F., and W.Z. fabricated the devices; E.S., Z.F., P.B., and C.O. carried out the measurements under the primary supervision of J.A.F. and D.H.C. in a cryostat developed by E.S., S.L., and J.A.F.; all authors contributed to the analysis of the data; E.S., J.A.F., and D.H.C. wrote the manuscript; all authors contributed to the final editing of the manuscript. Competing interests: The authors declare no competing interests. Data and materials availability: The data shown in the paper are available at

Stay Connected to Science

Navigate This Article