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Gated tuned superconductivity and phonon softening in monolayer and bilayer MoS2

npj Quantum Materialsvolume 2, Article number: 52 (2017) | Download Citation


Superconductors at the atomic two-dimensional limit are the focus of an enduring fascination in the condensed matter community. This is because, with reduced dimensions, the effects of disorders, fluctuations, and correlations in superconductors become particularly prominent at the atomic two-dimensional limit; thus such superconductors provide opportunities to tackle tough theoretical and experimental challenges. Here, based on the observation of ultrathin two-dimensional superconductivity in monolayer and bilayer molybdenum disulfide (MoS2) with electric-double-layer gating, we found that the critical sheet carrier density required to achieve superconductivity in a monolayer MoS2 flake can be as low as 0.55 × 1014 cm−2, which is much lower than those values in the bilayer and thicker cases in previous report and also our own observations. Further comparison of the phonon dispersion obtained by ab initio calculations indicated that the phonon softening of the acoustic modes around the M point plays a key role in the gate-induced superconductivity within the Bardeen–Cooper–Schrieffer theory framework. This result might help enrich the understanding of two-dimensional superconductivity with electric-double-layer gating.


Discovery of the interfacial superconducting state at the atomic scale has motivated the pursuit of emergent condensed phases in two-dimensional (2D) electronic systems. Studies of interfacial superconductivity have been generally limited to the regime in which the superconducting order parameter is restricted to 2D. Examples include one-atomic-layer Pb or In films on a Si (111) substrate,1,2,3,4,5 single-unit-cell FeSe films on a SrTiO3 substrate6,7,8,9 and few layer NbSe2 crystal.10, 11 Recent advances in electric-double-layer (EDL) gating have enabled the continuous tuning of one of the order parameters—the superfluid density—in 2D superconductors on the surface of bulk crystals with unprecedented control of surface band bending, doping level and vortex interaction, thus opening up new opportunities for understanding 2D superconductivity in the surface accumulation layers.12,13,14,15,16,17,18 With the reduced dimensionality—especially in a strict 2D monolayer form in layered materials in which the disorder, fluctuation and correlation effects all play particularly important roles—being the key parameter, how low the carrier density can be to realize the interfacial superconductivity approaching the ultimate atomic limit remains elusive.

Therefore, to investigate the superconductivity at the monolayer limit starts to be a topic of great interest.18 As a representative semiconducting layered material, monolayer and bilayer MoS2 (Fig. 1a) was chosen here as an ideal platform to study superconductivity at its 2D limit because of the following advantages: (1) The dramatic change in the band structure once the crystal is thinned down from bilayer to monolayer provides us with the possibility to understand the effect of some specific subband structures and Fermi surfaces on the superconductivity; (2) The unique electric-field-driven Zeeman splitting16, 19, 20 in the valleys of conduction bands might potentially provide spin-valley locking or a triplet electron pairing mechanism in the unique band structure of monolayer MoS2;21 and (3) Technically, relatively clean atomically thin monolayer and bilayer flakes are easily accessible by using mechanical cleavage. In addition, combined with the powerful accessibility of the EDL gating technique, superconductivity in monolayer and bilayer MoS2 can help us achieve a deep understanding of the microscopic mechanism of 2D superconductivity. Recently, Costanzo et al.18 used this technique to study the superconductivity in thin MoS2 flakes with thickness ranging from mono-layer to six-layers.

Fig. 1
Fig. 1

Crystal structure, device geometry, and gate-induced superconductivity of monolayer and bilayer MoS2 EDLT devices. a Crystal structure of 2H-MoS2, where the interlayer spacing is 0.615 nm. b Optical microscope image of a typical bilayer MoS2 EDLT device. Scale bar: 20 μm. c Schematic illustration of an atomically thin MoS2 EDLT device. The labels of S and D represent source and drain electrodes, respectively. d Typical ambipolar transfer curves obtained from a bilayer MoS2 EDLT device at 220 K (blue: forward direction; red: backward direction). V DS was fixed at 10 mV. e, f T-dependent R s of bilayer (e) and monolayer (f) MoS2 devices at different perpendicular magnetic fields showing gate-induced superconductivity

In this work, we also demonstrated gate-induced 2D superconductivity in monolayer and bilayer MoS2 in an electric-double-layer transistor (EDLT) geometry and we found that the monolayer sample showed a smaller critical sheet carrier density requirement to achieve superconductivity than those of bilayer and bulk samples. The comparison studies of their vortex motions on monolayer and bilayer superconductivity were conducted to gain an insight into the differences in the microscopic pictures of the 2D superconductivity. Our further ab initio calculations identified that the superconductivity are mainly induced by the phonon-softening of in-plane acoustic phonon modes and via such a mechanism the monolayer MoS2 can be more easily driven into superconducting phase with the less electron doping compared to the bilayer case. This work might enrich the understanding of gated interfacial superconductivity approaching the ultimate atomic limit and provides a method to achieve new types of superconductors.


Figures 1b, c show the typical device structure (optical image) and measurement geometry (schematic illustration) of EDLT using an ionic liquid (DEME–TFSI) as the gate medium. Due to the large tunability of the chemical potential using EDLTs, Fig. 1d presents an ambipolar operation of bilayer MoS2 EDLT devices at 220 K with an ON–OFF ratio of 105 and a maximum attainable sheet carrier density (n) up to ~2 × 1014 cm−2 by applying sufficiently high gate voltage V LG via the EDL gating medium. As shown in Fig. 1e, in a typical case of a bilayer MoS2 device with n = 1.3 × 1014 cm−2 (measured at 10 K), clear superconducting behavior can be observed. The superconducting state was gradually suppressed upon the application of an increasing perpendicular magnetic field and was completely suppressed when the magnetic field reached 1 T (see supplementary information for more details). In addition to the main drop in sheet resistance R s at 3.3 K, we noted two other small resistance drops at higher temperatures above the superconducting transition, which are likely caused by the slightly inhomogeneous carrier accumulation. These observations suggest that the inhomogeneity-induced fluctuation in the chemical potential of the channel could cause a more notable effect on the electron transport properties while approaching the 2D limit.

To examine the dimensionality nature of such EDL gating-induced superconductivity, we performed 4-probe voltage-current (VI) measurements and found that the results satisfied the Berezinskii–Kosterlitz–Thouless (BKT) transition22,23,24 (supplementary Figs. S3, S4) for 2D superconductivity. The BKT transition corresponds to the spontaneous dissociation of vortex-antivortex pairs into free vortices at the transition temperature T BKT. By fitting the VI and R sT curves, we obtained a transition temperature T BKT ~ 2 K (see supplementary Fig. S4 for more details). Compared with thicker MoS2 devices (~20 nm),14 enhancement of back gate modulation due to the atomically thin geometry was also observed (supplementary Fig. S5).

Superconductivity in a monolayer MoS2 flake is shown in Fig. 1f. The magnetic field response (shown in Fig. 1f) confirmed that the resistance drop during cooling-down is most likely the superconducting transition. Two remarkable characteristic features must be addressed here. First, before the transition to a superconductor, the resistance of both monolayer and bilayer flakes increases with decreasing temperature (more pronounced in the monolayer case), showing a stronger insulating behavior compared with that observed in thicker MoS2 flakes (20 nm).14 This result indicates that disorder plays a more important role in the 2D phase transition while approaching the thin limit. This disorder might originate from the inhomogeneous charge accumulation or the substrate effect on the channels. Second, the critical carrier density required to achieve the superconducting state in the monolayer case is much lower than those values observed in our bilayer case or reported thicker cases,14, 16, 20 which we will discuss in detail below. We note that due to the relatively small applied gate voltage to avoid possible electrochemical reactions and the limited temperature accessibility of our equipment, a zero resistance superconducting state was not reached. However, the interface effect between electrodes and sample,25, 26 finite-size effects24 and slightly inhomogeneous superconductivity15, 27 may also play roles in the non-zero resistance of low dimensional superconductivity. The bilayer superconductivities with zero resistance state under similar conditions suggest that the non-zero resistance case in monolayer MoS2 cannot be explained by finite-size effects or interface effect between electrodes and sample. The small applied gate voltage and slightly inhomogeneous superconductivity may be possible reasons and will require further investigations.

To study the detailed differences in the critical carrier densities required to achieve superconductivity between monolayer and bilayer MoS2, we first measured the low-temperature transport properties of bilayer devices at different carrier densities. Figure 2a shows the R sT curves (T = 200 to 1.6 K) of a different bilayer device (which is different to the one shown in Fig. 1e). With n = 0.95 × 1014 cm−2 (measured at 10 K with Hall effect results shown in the inset of Fig. 2a), the device remained metallic until a metal–insulator transition appeared at temperatures down to ~11 K, and no signature of superconductivity was observed. For the same devices, once the sheet carrier density n was increased slightly to ~1.23 × 1014 cm−2, a sharp R s drop emerged at temperatures of ~4.2 K, and the device reached a zero resistance state at ~1.55 K, indicating the occurrence of superconductivity. For a monolayer MoS2 device, however, a much smaller critical carrier density (~0.55 × 1014 cm−2, with the results shown in Fig. 2b) was observed than for those observed in bilayer devices. We summarize the main results in Fig. 2c, where T c [defined as R s(T c) = 0.9R s(10 K)] is plotted as a function of n for several typical devices (see a similar plot using number of carrier per primitive cell as the standard of the carrier density in Fig. S6, and additional data on homogeneity of carrier densities for multiple pairs of contacts in Fig. S7). All the carrier densities were determined by measuring Hall effect at 10 K, where the monolayer and bilayer MoS2 maintained normal states. The Hall resistance, R xy, show antisymmetric and linear characteristics when plot as a function of magnetic field (such as the inset of Fig. 2a, b). The negative sign of Rxy for positive magnetic field indicate electron-type carriers, which is consistent with the positive gate biases. And the carrier densities were extracted from the Hall coefficient R H for each gate voltage by using the formula \({R_{\rm{H}}} = 1{\rm{/}}ne\). Because disorders or fluctuations are generally believed to play a crucial role in disturbing the superconductivity upon approaching the 2D limit, it is counterintuitive to find that in the ultimate limit case (monolayer), it is “easier” to realize superconductivity than in the bilayer or bulk cases when tuning such a key parameter—carrier density n.

Fig. 2
Fig. 2

Comparison of critical carrier densities to achieve superconductivity in monolayer and bilayer MoS2. a Temperature-dependent resistance of a bilayer MoS2 EDLT at n = 0.95 × 1014 and 1.23 × 1014 cm−2. Inset: Hall measurement results. b Temperature-dependent resistance of a monolayer MoS2 EDLT at n = 0.55 × 1014 cm−2. Inset: Hall measurement results. c Critical temperature T c versus carrier density n for monolayer and bilayer MoS2. T c is defined as R s(T c) = 0.9R s(10 K)

Another approach to gain insight into the differences in the microscopic pictures of the 2D superconductivity in monolayer and bilayer MoS2 devices is to study their vortex motion.17 Through analysis of R sT plots under various perpendicular magnetic fields on typical bilayer (Fig. 3a) and monolayer (Fig. 3b) devices, we observed the activated behavior of the vortex dynamics at temperatures slightly lower than T c and at the resistance saturation at even lower temperatures. This behavior is similar to that recently observed in a ZrNCl EDLT superconductor17 and in disordered metal thin films.28 At temperatures slightly lower than T c, the sheet resistance can be described by

$${R_{\rm{S}}} = {R_0}(H){e^{ - \frac{{U\left( H \right)}}{{{k_{\rm{B}}}T}}}},$$

where U(H) is the activation energy, and k B is Boltzmann’s constant. The fitting (black dotted lines in Fig. 3a, b) yields values of U(H). We further plotted the dependence of U(H)/k B on H, as shown in Fig. 3c, and found that both monolayer and bilayer devices follow the relation of

$$U\left( H \right) = {U_0}{\rm{ln}}\left( {{H_0}{\rm{/}}H} \right),$$

where \({U_0}\sim {\Phi_0^2}d/256{\pi ^3}{\lambda ^2}\) represents the vortex–antivortex binding energy, Φ 0 is the flux quantum, d is the interlayer spacing, λ is the London penetration length depth, and H 0 ~ H c2 (defined as R s(H c2) = 0.9R s(10 K)). These results indicate that the vortices in both monolayer and bilayer devices exhibit thermally activated flux flow (TAFF).29 From the fitting results of the bilayer device, we obtained U 0/k B = 9.1 K and H 0 = 0.37 T (H 0 was found be smaller than H c2 in this device), which are much larger than those of the monolayer device (U 0/k B = 0.12 K and H 0 = 0.37 T). At lower temperatures, the resistance deviated from the thermally activated behavior, and a magnetic-field-induced metallic ground state emerged. For the bilayer device, we also measured the magnetic field dependence of R s at 0.3 K (see supplementary information for more details) and obtained a good fit (inset of Fig. 3c) by using a model developed by Shimshoni et al.30 and Saito et al.17 in the low magnetic field regime, indicating that the vortices move through quantum tunneling.

Fig. 3
Fig. 3

Vortex dynamics analysis of monolayer and bilayer MoS2. a and b show the Arrhenius plot of the sheet resistance of two typical bilayer and monolayer MoS2 EDLTs at different perpendicular magnetic fields, respectively. The dashed lines show the guide-to-eye fit of the thermally activated behavior, and the arrows show the deviation of the thermally activated regimes. c Semilogarithmic plot of the activation energy, U(H)/k B, as a function of magnetic field for both monolayer and bilayer devices. U(H)/k B data were extracted from fittings in Fig. 3a, b. The solid line is a fit to the formula U(H) = U 0ln(H 0/H). Inset: the magnetic field dependence of R s at 0.3 K with a fit obtained by using a model developed by Shimshoni et al.30 and Saito et al.17 d Vortex phase diagram of the bilayer and monolayer (inset) MoS2 EDLT devices. The solid circles represent H c2 at different temperatures, and the solid squares were extracted from the deviation points as shown in a and b (depicted by the black arrows). The solid squares divide the thermally activated flux flow (TAFF) and quantum creep regimes

The vortex phase diagrams of both monolayer and bilayer devices based on our observations are plotted in Fig. 3d. Two phases, the TAFF and quantum creep, are confirmed by the measured H c2 and thermally activated behavior deviation points. When temperatures drop below T c, the vortices move through the superconductor by thermal activation, whereas at even lower temperatures in a low magnetic field, vortices move by quantum tunneling. The movement of vortices indicates that even down to atomic thickness, the gate-induced 2D superconductor systems still reside in the weak disorder limit. In gate-induced superconductors in thick flakes of layered materials,17 the superfluid density is confined in a few layers near the surface, and the 2D superconductors are susceptible only to relatively weak disorder generated by random electric potential from the ions; thus, they exhibit the behavior of a clean 2D superconductor. Herein, the monolayer and bilayer MoS2 flakes are exfoliated onto SiO2 wafers, so the 2D superconductor is affected by stronger disorder from the substrate in addition to the ionic liquid. It is worth noting that these systems remain in a regime of a disordered 2D superconductor.

A quantum metallic state was also observed in bilayer NbSe2 crystal covered by Boron nitride (BN).11 The low temperature resistance of the state fulfills a power-law scaling with magnetic field, which is consistent with the so-called Bose-metal model. This mainly attributes to the covered BN which protects NbSe2 crystal from the influence of atmosphere, resulting in a nearly disorder-free condition. While in the case of thin MoS2 flakes, related EDLT systems remain in the disordered regime where quantum creep is expected to depict the quantum metallic state.17 This explains why the low temperature resistance of these two systems exhibits different magnetic field dependence. For the quantum metallic state of NbSe2 systems, it originates from the magnetic field induced strong phase fluctuations. Nevertheless, for the MoS2 EDLT systems, magnetic-field-induced vortices move through quantum tunneling yields a different metallic ground state. More efforts should be involved to further understand the vortex dynamics of the MoS2 EDLT systems.


To fully understand the physical mechanism of 2D superconducting varying with carrier density, we perform ab initio density functional theory (DFT) calculations for the electronic structures of electron-doped monolayer and bilayer MoS2. We choose several doping levels (from 0.57 × 1014 to 2.74 × 1014 cm−2) to simulate the accumulated carrier density achieved in the liquid gating experiment, which is unavailable for conventional oxide-gated samples. It should be noted here that the electronic band structures of doped monolayer and bilayer MoS2 strongly depend on the charge doping as shown in Fig. 4a, d. Consistent with previous Angle-resolved photoemission spectroscopy measurement,31 the conduction band minima of monolayer and bilayer MoS2 are always located at the K (K′) point even when electrons are injected into the samples. With increasing doping level, the conduction band edge at the K (K′) point is filled, and the relative energy difference between the conduction band edge at the K (K′) and Λ (Λ′) points becomes smaller. By further increasing the electron doping, the states at the Λ (Λ′) points are filled, whose energy splitting induced by the spin orbital coupling is much larger than that at the K (K′) point.32 Therefore, the electronic Fermi surface of the heavily doped MoS2 contains two parts: one is around the K and K′ points, and the other is located near the Λ and Λ′ points. This result directly suggests that the electronic states around the Λ and Λ′ points have a greater chance to be paired to form superconducting states via the phonon modes once the carrier density is sufficiently high to induce superconductivity in this system (as discussed below), which is different from previous reports.20

Fig. 4
Fig. 4

Calculated electronic structures and electron-phonon couplings for the doped monolayer and bilayer MoS2. The band structures of a monolayer and d bilayer MoS2 with different doping levels. The Fermi level is set to zero and marked by black dotted lines. For the un-doped case, we set the energy of the conduction band minimum to zero. The phonon dispersion and the Eliashberg spectral functional for b, c monolayer and e, f bilayer MoS2 with different doping levels. Herein, LA, TA and ZA stand for in-plane longitudinal mode, in-plane transverse mode and out-plane transverse mode. For bilayer MoS2, the polarizations of these pairs of acoustic branches are denoted as follows: LA1/LA2, TA1/TA2 and ZA1/ZA2

In the framework of Bardeen–Cooper–Schrieffer theory, the superconducting T c is mainly determined by the electron–phonon coupling;33 the averaged coupling constant has the expression of

$$\lambda = 2{\int} {d\omega \frac{{{\alpha ^2}F\left( \omega \right)}}{\omega }} = \mathop {\sum}\limits_{{\boldsymbol{q}},\upsilon } {\frac{{2{\gamma _{{\boldsymbol{q}},\upsilon }}}}{{hN({{{\epsilon }}_{F}})\omega _{{\boldsymbol{q}},{\upsilon^2}}}}} ,$$

where \({\alpha ^2}F(\omega )\) is the Eliashberg spectral functional, \(N({{{\epsilon }}_F})\) is the electronic density of states at the Fermi level, \({\omega _{{\boldsymbol{q}},\upsilon }}\) is the phonon frequency, and \({\gamma _{{\boldsymbol{q}},\upsilon }}\) is the phonon line width (see the Methods section). Thus, herein, by using density functional perturbation theory (DFPT),34 we calculated the phonon bands and electron-phonon coupling for monolayer MoS2 with different doping levels as shown in Fig. 4b, c. Toward the low-frequency part of the acoustic phonons that mainly contributes to superconductivity, the phonon softening of longitudinal and transverse acoustic phonon modes (LA and TA modes) is found around the M point with low carrier density (blue line in Fig. 4b); with increasing electron doping, the LA and TA modes can be further softened around the K point. This effect occurs because the electronic states around the Λ (Λ′) point are filled at higher doping levels. However, for the whole calculated doping range, the out-of-plane mode (ZA mode), \(N({{{\epsilon }}_{\rm{F}}})\) and \({\gamma _{q,\upsilon }}\) change little (see supplementary information for more details). Thus, we conclude that the gate-induced superconductivity for the doped monolayer MoS2 originates from the phonon softening of low-frequency TA and LA modes at the K and M points, and this result is further confirmed by the \({\alpha ^2}F(\omega )\) calculations (see Fig. 4c).

In contrast to monolayer MoS2 superconductivity, the accumulated carrier density of a doped bilayer is lower for the same magnitude of T c, which is observed experimentally in Fig. 2c. These phenomena are confirmed by our DFPT calculations. In Fig. 4e, f, we show the calculated phonon dispersions and electron–phonon couplings for doped bilayer MoS2. It is found that although the phonon softening also occurs at the M and K (K′) points, the magnitude is much weaker in bilayer MoS2 at the same doping level, which indicates that superconductivity in the bilayer or multilayer MoS2 is more difficult to achieve due to the interlayer coupling. In experimental reality, the influence of the substrate and fluctuations in and inhomogeneity of the electron distribution also play important roles for 2D superconducting, which is still an open question and cannot be captured by our DFT calculations.

In conclusion, we demonstrate that in the gate-induced 2D superconductivity of both monolayer and bilayer MoS2 flakes, the monolayer sample has an apparently smaller critical sheet carrier density to achieve superconductivity than those of bilayer and bulk samples. The ab initio calculation results point to the phonon softening of in-plane acoustic phonon modes as a possible origin of these observations. Our work paves the way for further understanding of gated interfacial superconductivity approaching the ultimate atomic limit and pursuing a new type of superconductor.


Materials and devices

The monolayer and bilayer MoS2 flakes on silicon wafers (covered by 300-nm-thick SiO2) were fabricated by standard mechanical exfoliation of bulk MoS2 (SPI supplies). The number of layers was determined by measuring the thickness of the flakes using a Bruker Multimode 8 atomic force microscope or performing micro Raman scattering (Horiba-JY T64000) measurements (under ambient conditions in the backscattering geometry with an incident laser wavelength of 514.5 nm). A conventional electron-beam lithography process (FEI F50 with an NPGS pattern generation system) followed by standard electron-beam evaporation of metal electrodes (typically 5 nm Ag/ 40 nm Au) was used to fabricate Hall bar electrodes.

Transport measurements

The ionic liquid used in this study was N,N-diethyl-N-(2-methoxyethyl) -N-methylammonium bis-(trifluoromethylsulfonyl)-imide (DEME–TFSI). An ionic liquid drop was applied onto MoS2 devices with Hall geometry and covered both the MoS2 flake and a side gate electrode to form an EDLT. Before any electrical measurements were performed, the MoS2 EDLT devices were stored under a vacuum better than 10−2 mbar and cooled down to 220 K to avoid possible interfacial chemical reactions.

The transport measurements of all MoS2 EDLTs were performed in an Oxford Instruments TeslatronTM CF cryostat. Due to the freezing of the ionic liquid at low temperatures, we applied different values of V LG to accumulate carriers of certain density at 220 K and cooled down with a fixed V LG. A lock-in amplifier (Stanford Research 830) was used to measure the 4-probe resistance through the AC approach.

Ab initio calculations

The ab initio calculations were performed by using DFT as implemented in the Quantum Espresso35 package. For the electronic structure calculations, the 32 × 32 × 1 Monkhorst-Pack k points were used with the generalized gradient approximation (GGA) functional36 and norm-conserving pseudopotential. To correctly describe the electronic structures of monolayer and bilayer MoS2 and repeat the previous calculations,31 the in-plane lattice constant was chosen as 3.18 Å; the vacuum layer was chosen as 15 Å that was sufficiently large to avoid the interaction between adjacent layers, and inner coordinates of unit-cell were fully relaxed. Phonon band structures and electron–phonon couplings were calculated within DEPT34 based on the evaluation of the dynamical matrices on the 8 × 8 × 1 q-mesh. For the phonon dispersion, SOC was not considered.

Data availability

The data that support the findings of this study are available from the corresponding author upon reasonable request.

Additional information

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This work was supported in part by the National Key Basic Research Program of China (2015CB921600, 2013CBA01603), the National Natural Science Foundation of China (11374142, 61574076), the Natural Science Foundation of Jiangsu Province (BK20130544, BK20140017, BK20150055), the Specialized Research Fund for the Doctoral Program of Higher Education (20130091120040), and Fundamental Research Funds for the Central Universities and the Collaborative Innovation Center of Advanced Microstructures. This work was partially supported by the Department of Energy, Office of Basic Energy Sciences, Division of Materials Sciences and Engineering, under contract DE-AC02-76SF00515. P.Z.T., B.L., G.X. and S.C.Z. also acknowledge NSF under grant number DMR-1305677.

Author information

Author notes

  1. Yajun Fu, Erfu Liu, Hongtao Yuan and Peizhe Tang contributed equally to this work


  1. National Laboratory of Solid State Microstructures, School of Physics, Collaborative Innovation Center of Advanced Microstructures, Nanjing University, Nanjing, 210093, China

    • Yajun Fu
    • , Erfu Liu
    • , Junwen Zeng
    • , Yaojia Wang
    • , Wei Zhou
    • , Kang Xu
    • , Anyuan Gao
    • , Chen Pan
    • , Miao Wang
    • , Baigeng Wang
    •  & Feng Miao
  2. Stanford Institute for Materials and Energy Sciences, SLAC National Accelerator Laboratory, Menlo Park, CA, 94025, USA

    • Hongtao Yuan
    • , Shou-Cheng Zhang
    • , Yi Cui
    •  & Harold Y. Hwang
  3. Geballe Laboratory for Advanced Materials, Stanford University, Stanford, CA, 94305, USA

    • Hongtao Yuan
    • , Peizhe Tang
    • , Biao Lian
    • , Gang Xu
    • , Zhuoyu Chen
    • , Shou-Cheng Zhang
    • , Yi Cui
    •  & Harold Y. Hwang


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Y.J. F., E.F. L., H.T. Y. and P.Z. T. contributed equally to this work. F. M. and H.T. Y. conceived the project and designed the experiments. Y.J. F., E.F. L., J.W. Z., Y.J. W., W. Z., K. X., A.Y. G., C. P., and M. W. performed device fabrication, characterization and transport measurements. Y.J. F., E.F. L., F. M. and H.T. Y. performed data analysis and interpretation. P.Z. T., B. L., X. G., Z.Y. C. and S.C. Z. performed DFT calculations. H.T. Y., F. M., Y.J. F. and E.F. L. co-wrote the paper, and all authors contributed to the discussion and preparation of the manuscript.

Competing interests

The authors declare that they have no competing financial interests.

Corresponding authors

Correspondence to Hongtao Yuan or Baigeng Wang or Feng Miao.

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