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Superconductivity from the Slater mode: Application to KTaO3 heterostructures

T0 review · 0 major / 5 minor · reviewed 2026-08-03 · deepseek-v4-flash

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Pith's one-line read Pairing through the soft Slater phonon reproduces the orientation dependence of superconductivity in KTaO3 interfaces, but cannot alone produce the observed Tc.

desk verdict A credible microscopic application of Slater-mode pairing to KTO interfaces, with an honest negative result on λ; the orientation hierarchy is likely robust, but the forward-scattering kernel rests on a vertex assumption worth checking. read the letter →

arxiv 2601.10903 v2 pith:NOHF7NPG submitted 2026-01-15 cond-mat.supr-con

M. R. Norman This is my paper · ORCID
classification cond-mat.supr-con
keywords KTaO3superconductivity2DelectrongasSlatermodeelectron-phononcouplingRashbaquantumparaelectricoxideheterostructure
verification ladder T0 review T1 audit T2 compute T3 formal

The pith

A machine-rendered reading of the paper's core claim, the machinery that carries it, and where it could break.

The reading

This paper tests whether the soft transverse-optic (Slater) phonon—the mode that drives ferroelectricity in quantum paraelectrics—can explain the superconductivity observed in the two-dimensional electron gas at KTaO3 heterostructures. Pairing is mediated by phonon-induced Rashba couplings computed from first principles, and the linearized gap equation is solved for (111) and (001) interfaces using two tight-binding models. The computed BCS coupling constant λ is much larger for (111) than for (001), matching the measured ordering of transition temperatures, and the gap function is strongly anisotropic in band index and Fermi-surface angle. However, for realistic parameters λ is about 0.05, far below the roughly 0.26 needed for a Tc near 2 K, so the Slater mode alone cannot account for the absolute magnitude of Tc. The paper concludes that other phonons must add to the pairing.

What carries the argument

The load-bearing object is the dynamic Rashba electron-phonon coupling generated by the TO1 (Slater) mode: phonon-induced hoppings among t2g orbitals via oxygen 2p states, with one spin-independent term (t0) and three spin-dependent terms (tA, tB, tC) taken from first-principles calculations. In the Cooper channel these couplings act at the average momentum k0 = (k+k')/2, which makes the pairing interaction peak at forward scattering and vanish at back scattering. The gap equation is built as a secular matrix whose kernel combines these matrix elements with the Vaks-parameterized phonon dispersion ω(q); solving the linearized gap equation yields the BCS constant λ and the order parameter Δnk

What would settle it

Measure the superconducting gap anisotropy on a (111) KTaO3 interface by tunneling: the calculation predicts a gap Δnk that varies strongly with band index and Fermi-surface angle, peaking in specific directions tied to the star-shaped Fermi surface. A gap that is essentially isotropic, or a Tc(111)/Tc(001) ratio that disagrees with the computed λ ratio while other phonon contributions are held fixed, would rule out the Slater mode as the dominant pairing agent.

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Extended reading notes

Core claim

The central claim is that the soft TO1 (Slater) phonon, acting through dynamic Rashba couplings, is a major contributor to the superconductivity of the KTaO3 two-dimensional electron gas and explains why the (111) interface has a much higher Tc than the (001) interface. Solving the linearized gap equation in a bilayer tight-binding model, the paper finds λ111 ≈ 0.04–0.13 and λ001 ≈ 0.001–0.01 (depending on the tight-binding model and phonon dispersion), reproducing the orientation hierarchy observed in experiment. The gap function Δnk varies significantly with band index and Fermi-surface angle. The same calculation gives λ values well below the ~0.26 needed for the observed Tc ≈ 2 K at n2D

Load-bearing premise

The computation assumes the dynamic Rashba couplings derived for bulk KTaO3 apply unchanged at the interface, apart from a geometric 1/√3 factor for the (111) polarization; altered screening, confinement, or structural relaxation at the interface would change the computed λ and the absolute conclusion about Tc.

Editorial extensions

If this is right

  • The orientation hierarchy T111 > T110 > T001 in KTaO3 interfaces follows from the orbital degeneracy of the t2g manifold and the projection of the Slater-mode polarization, giving a concrete orbital-based design rule for enhancing Tc.
  • The predicted strong band-index and in-plane angular dependence of the superconducting gap is observable by tunneling spectroscopy, providing a direct fingerprint of Slater-mode pairing.
  • Because λ scales roughly as 1/ω(0) when the phonon dispersion is included, experiments that soften the TO1 mode—such as doping toward the ferroelectric quantum critical point—should raise Tc substantially.
  • The finding that the Slater mode alone gives λ ≈ 0.05 implies that other phonons, especially orientation-dependent high-energy modes, must contribute to reach the observed Tc values; theories focusing only on the Slater mode will underestimate Tc.
  • The strong forward-scattering peak suggests that pairing at these interfaces is dominated by small-momentum-transfer processes, which may favor unconventional gap structures.

Reading between the lines

Editorial extensions of the paper, not claims the author makes directly.

  • If the orientation hierarchy is as robust as argued, engineering the confinement potential—via gate voltage or capping layers—to change orbital occupancy could provide a tunable knob for Tc across interfaces, a testable extension beyond the paper's numbers.
  • The reliance on bulk-derived dynamic Rashba couplings at the interface is the natural place for a more complete heterostructure calculation (coupled Schrödinger–Poisson plus interface screening) to improve the quantitative estimate of λ.
  • The forward-scattering nature of the interaction raises the possibility that in higher-order channels or under stronger coupling the gap could develop nodes or even pair-density-wave character; tunneling and specific-heat measurements could look for this.
  • If the Slater-mode contribution is supplemented by other phonons, combined isotope-effect experiments or terahertz/inelastic-neutron studies of the interfacial phonon spectrum would help decide which modes matter.
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Editorial analysis

A structured set of objections, weighed in public.

Desk editor's note, referee report, and a circularity audit.

Referee Report

0 major / 5 minor

Summary. The paper studies superconductivity in the 2DEG at KTaO3 interfaces driven by the soft transverse optic (TO1 or Slater) phonon mode. Starting from a microscopic theory of the dynamic Rashba electron-phonon coupling (Gastiasoro et al., Phys. Rev. B 105, 224503) and ab-initio couplings for bulk KTO (Venditti et al., arXiv:2510.25655), the author constructs a linearized gap equation for a bilayer tight-binding model of the (111) and (001) interfaces. The secular matrix includes the four dynamic Rashba terms and the q-dependent TO1 phonon dispersion. The numerical solutions yield the BCS coupling constant λ and the angular- and band-dependent gap function. The main results are: (1) λ for (111) exceeds that for (001) by one to two orders of magnitude for all parameter choices, consistent with the observed orientation dependence of Tc; (2) the gap function is strongly anisotropic and band-dependent; and (3) λ for (111) is at most ~0.13, well below the ~0.26 needed for Tc≈2 K, indicating that the Slater mode alone cannot account for the absolute Tc and other phonons must contribute. The paper is transparent about the approximations and lists possible improvements.

Significance. This is a valuable contribution that puts the phenomenological Slater-mode pairing scenario on a concrete microscopic footing for KTO interfaces. The calculation uses published ab-initio couplings and two tight-binding models, and no parameter is fitted to Tc; the orientation hierarchy is robust across these choices. The explicit gap-function anisotropy is a new prediction that could be tested by tunneling. The honest reporting that the Slater mode alone gives λ too small is an important negative result, narrowing the search for the pairing glue. The main limitations—interface transferability of the bulk couplings, the static-phonon approximation, and the neglect of other phonon modes—are clearly acknowledged. If the results hold, they will likely steer future work toward including LO phonons and full strong-coupling calculations.

minor comments (5)
  1. [Section II, Eq. (3)] The statement that the dynamic Rashba matrix elements are evaluated at k0=(k+k')/2 is important because it suppresses back-scattering, but it is not derived. The stress-test concern that the vertex might depend on the incoming momentum is addressed by the standard symmetrization of a local coupling (the coupling α(x) p·σ yields a vertex proportional to (k+k')/2), but this should be stated explicitly, with a reference to the specific equation in Ref. [11]. Please add a short derivation or an explicit citation.
  2. [Section III (111 case)] The 1/√3 scaling of t_i for the (111) polarization is stated without derivation. Since this factor directly affects λ_111 and hence the central quantitative claim, please show the projection of the phonon eigenvector onto the coupling tensor. Also, consider a brief comment on whether the same projection applies to all four t_i terms.
  3. [Eq. (3)] The use of the static phonon propagator with a q-dependent energy is a hybrid approximation; a one-sentence justification in terms of the adiabatic parameter ω(2k_F)/E_F would be helpful.
  4. [Table III and Fig. 5] The labels 'ω(q)' and 'ω(0)' in the table and figure headers are clear in context, but a fuller caption or a note in the text defining the abbreviation (e.g., 'ω(q) means the full Vaks dispersion is used') would improve readability.
  5. [Throughout] Minor typos: 'can by thought of' should be 'can be thought of' in Section II; 'Rasbha' should be 'Rashba' in the text before Table II; spacing in Eq. (3) is irregular.

Circularity Check

0 steps flagged · score 0.0 of 10

No significant circularity: λ values are computed from ab initio dynamic Rashba couplings with no fit to Tc or orientation data.

full rationale

The derivation chain is self-contained. The central quantities (Table III λ's) come from solving the linearized gap equation, Eq. 3, using dynamic Rashba matrix elements taken from external ab initio work (Ref. [12]) and a TO1 phonon dispersion tied to neutron/Raman data (Refs. [25,26]). No parameter is adjusted to reproduce the observed Tc or the 111/001 ratio. The conclusion that λ is too small (≈0.05 vs ≈0.26 needed) is a computed mismatch, not an input. The orientation dependence of λ follows from the orbital structure of two tight-binding models anchored to ARPES and DFT (Refs. [14,15,19]) and from the physical projection of the TO1 polarization; the explicit 1/√3 reduction of the 111 couplings actually works against the hierarchy, making the computed 111/001 ratio a non-trivial result. Self-citations to Ref. [9] provide context, the Vaks phonon parameterization, and the ω(0)=5.6 meV screening estimate, but those inputs are grounded in external Raman and neutron data, so they are independent support rather than circular self-support. The evaluation of the dynamic Rashba vertex at k0=(k+k')/2 is a stated modeling assumption inherited from Ref. [11] (not a self-citation); if this vertex choice is wrong it would change the magnitude of λ, but that is a correctness risk, not a circular step. The paper also explicitly lists missing contributions (Discussion, items 1–6), further showing that the central negative result is not constructed from its own output.

Assumptions & free parameters 2 free parameters · 6 assumptions · 0 invented entities

The calculation relies on a chain of inputs from prior literature (ab-initio couplings, tight-binding parameters, Vaks phonon dispersion) and on several modeling assumptions that are explicitly acknowledged. The central result—the orientation hierarchy of λ—is robust to reasonable variations, but the absolute λ depends on ω(0) and on the transfer of bulk coupling values to the interface.

free parameters (2)
  • TO1 mode energy at q=0, ω(0) = 5.6 meV (estimated; 2.5 meV also used)
    The soft mode energy enters the phonon propagator in Eq. 3 and sets λ ∝ 1/ω(0). It is estimated from a screening model (Appendix B) rather than measured at the interface. The paper tests both 2.5 and 5.6 meV; λ varies by roughly a factor of 2.4.
  • Static Rashba coupling, t0_static = 2 meV
    A small static Rashba term is introduced by hand to lift Kramers degeneracy and define the band structure used in the gap equation (Section II and Fig. 1). It is not fitted to superconductivity and is much smaller than the dynamic coupling.
assumptions (6)
  • domain assumption Rashba-mediated pairing Hamiltonian and secular equation from Ref. [11]
    The core pairing interaction and the form of the linearized gap equation are adopted from prior work on bulk incipient ferroelectrics.
  • domain assumption Bilayer approximation for the interface electronic structure
    The interface 2DEG is modeled as a single bilayer, which reproduces ARPES star-shaped Fermi surfaces but ignores self-consistent confinement effects (acknowledged in Discussion item 6).
  • domain assumption Static approximation for the phonon propagator
    The phonon propagator is taken as -2/ω(q), ignoring retardation (Section II: 'we assume as in Ref. [11] a static approximation').
  • domain assumption Only the TO1 mode polarized perpendicular to the interface couples
    Coupling to the in-plane polarized TO1 mode is neglected, argued to be small from a circular Fermi surface argument (Section II).
  • domain assumption Gap transforms under the identity representation
    The order parameter is assumed to be invariant under the surface group operations (Section II: 'we assume it comes from the identity representation').
  • domain assumption Vaks parameterization of the TO1 phonon dispersion
    The q-dependent phonon energy ω(q) is taken from a parameterization of neutron scattering data (Ref. [25]), which is an empirical input.

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Cite this review

Pith. "Pith review of Superconductivity from the Slater mode: Application to KTaO3 heterostructures." pith.science (2026). https://pith.science/paper/NOHF7NPG

@misc{pith2026260110903,
  author       = {Pith},
  title        = {Pith review of: Superconductivity from the Slater mode: Application to KTaO3 heterostructures},
  year         = {2026},
  howpublished = {\url{https://pith.science/paper/NOHF7NPG}},
  note         = {Machine review of arXiv:2601.10903}
}
read the original abstract

Superconductivity has been observed for the 2D electron gas (2DEG) at the interface of KTaO3 with other oxides, with a transition temperature about an order of magnitude higher than its 3d cousin SrTiO3. The superconducting transition temperature is strongly dependent on the orientation of the interface. Motivated by this observation, we study pairing due to exchange of the soft transverse optic phonon mode characteristic of quantum paraelectrics and use the resulting theory to comment on the nature of superconductivity of this 2DEG. We find (1) an orientation dependence consistent with experiment along with an anisotropic gap function, but (2) a BCS coupling constant that is smaller than needed and so must be augmented by contributions from other phonons to be consistent with the observed values of Tc.

Figures

Figures reproduced from arXiv: 2601.10903 by the authors.

Figure 1
Figure 1. FIG. 1. Fermi surface for the bilayer 111 tight binding model [PITH_FULL_IMAGE:figures/full_fig_p004_1.png] view at source ↗
Figure 2
Figure 2. is exactly the effect mentioned above, where the kernel peaks for forward scattering (ϕ ′ − ϕ = 0) and is strongly suppressed for back scattering (ϕ ′ − ϕ = 180). There are two contributions to this, one coming from VR which has a tendency to peak either at or near forward scattering (top plots), and the additional contribution in brackets from the phonon dispersion where ω(q) has its lowest energy for forward scatt… view at source ↗
Figure 3
Figure 3. FIG. 3. Phonon dispersion [PITH_FULL_IMAGE:figures/full_fig_p004_3.png] view at source ↗
Figures from the paper (6 more)
Figure 6
Figure 6. Figure 6: FIG. 6. Fermi surface for the bilayer 111 tight binding model [PITH_FULL_IMAGE:figures/full_fig_p005_6.png]
Figure 4
Figure 4. Figure 4: FIG. 4. Plots of Eq [PITH_FULL_IMAGE:figures/full_fig_p005_4.png]
Figure 7
Figure 7. Figure 7: FIG. 7. The superconducting order parameter ∆ [PITH_FULL_IMAGE:figures/full_fig_p005_7.png]
Figure 10
Figure 10. Figure 10: FIG. 10. The superconducting order parameter ∆ [PITH_FULL_IMAGE:figures/full_fig_p006_10.png]
Figure 11
Figure 11. Figure 11: FIG. 11. Variation of the BCS coupling constant [PITH_FULL_IMAGE:figures/full_fig_p006_11.png]
Figure 9
Figure 9. Figure 9: FIG. 9. Plots of Eq [PITH_FULL_IMAGE:figures/full_fig_p006_9.png]

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Works this paper leans on

34 extracted references · 1 canonical work pages

  1. [11]

    In a simple approximation where the Fermi surface is circular, this vanishes in that ⃗k0 is trans- verse to⃗ q

    goes as ⃗k0 ·⃗ q. In a simple approximation where the Fermi surface is circular, this vanishes in that ⃗k0 is trans- verse to⃗ q. So, we expect in general that coupling to this mode is small and so we ignore it, though a more com- plete calculation than what we present here would take it into account. Finally, the form of Eq. 3 implicitly assumes that ∆ n...

  2. [1]

    Ohtomo and H

    A. Ohtomo and H. Y. Hwang, A high-mobility electron gas at the LaAlO 3/SrTiO3 heterointerface, Nature427, 423 (2004)

    2004

  3. [2]

    Reyren, S

    N. Reyren, S. Thiel, A. D. Caviglia, L. F. Kourkoutis, G. Hammerl, C. Richter, C. W. Schneider, T. Kopp, A.- S. R¨ uetschi, D. Jaccard, M. Gabay, D. A. Muller, J.-M. Triscone, and J. Mannhart, Superconducting interfaces between insulating oxides, Science317, 1196 (2007)

    2007

  4. [3]

    J. F. Schooley, W. R. Hosler, and M. L. Cohen, Super- conductivity in semiconducting SrTiO3, Phys. Rev. Lett. 12, 474 (1964)

    1964

  5. [4]

    J. M. Edge, Y. Kedem, U. Aschauer, N. A. Spaldin, and A. V. Balatsky, Quantum critical origin of the supercon- ducting dome in SrTiO 3, Phys. Rev. Lett.115, 247002 (2015)

    2015

  6. [5]

    K. Ueno, S. Nakamura, H. Shimotani, H. Yuan, N. Kimura, T. Nojima, H. Aoki, Y. Iwasa, and M. Kawasaki, Discovery of superconductivity in KTaO 3 by electrostatic carrier doping, Nature Nanotechnology 6, 408 (2011)

    2011

  7. [6]

    C. Liu, X. Yan, D. Jin, Y. Ma, H.-W. Hsiao, Y. Lin, T. M. Bretz-Sullivan, X. Zhou, J. Pearson, B. Fisher, J. S. Jiang, W. Han, J.-M. Zuo, J. Wen, D. D. 9 Fong, J. Sun, H. Zhou, and A. Bhattacharya, Two- dimensional superconductivity and anisotropic transport at KTaO 3 (111) interfaces, Science371, 716 (2021), https://www.science.org/doi/pdf/10.1126/scienc...

    doi:10.1126/science.aba5511 2021

  8. [7]

    Z. Chen, Z. Liu, Y. Sun, X. Chen, Y. Liu, H. Zhang, H. Li, M. Zhang, S. Hong, T. Ren, C. Zhang, H. Tian, Y. Zhou, J. Sun, and Y. Xie, Two-dimensional supercon- ductivity at the LaAlO 3/KTaO3 (110) heterointerface, Phys. Rev. Lett.126, 026802 (2021)

    2021

Show all 34 references
  1. [8]

    J. Kim, M. Yu, A. Omran, J. Yang, R. Ramachandran, W. O. Nachlas, P. Irvin, J. Levy, and C.-B. Eom, En- hanced superconductivity at quantum-critical KTaO3 in- terfaces (2025), arXiv:2511.12904 [cond-mat.supr-con]

    2025

  2. [9]

    C. Liu, X. Zhou, D. Hong, B. Fisher, H. Zheng, J. Pearson, J. S. Jiang, D. Jin, M. R. Norman, and A. Bhattacharya, Tunable superconductivity and its ori- gin at KTaO3 interfaces, Nature Communications14, 951 (2023)

    2023

  3. [10]

    Yang and L

    F. Yang and L. Q. Chen, Ferroelectric order and enhanced interfacial superconductivity in lightly- doped quantum paraelectric KTa 1−xNbxO3 (2025), arXiv:2511.08253 [cond-mat.mtrl-sci]

    2025

  4. [12]

    Venditti, F

    G. Venditti, F. Macheda, P. Barone, J. Lorenzana, and M. N. Gastiasoro, Spin-dependent anisotropic electron- phonon coupling in KTaO 3 (2025), arXiv:2510.25655 [cond-mat.mtrl-sci]

    2025

  5. [13]

    M. N. Gastiasoro, M. E. Temperini, P. Barone, and J. Lorenzana, Theory of superconductivity mediated by Rashba coupling in incipient ferroelectrics, Phys. Rev. B 105, 224503 (2022)

    2022

  6. [14]

    Villar Arribi, A

    P. Villar Arribi, A. Paramekanti, and M. R. Norman, Striped electron fluid on (111) KTaO3, Phys. Rev. B103, 035115 (2021)

    2021

  7. [15]

    X. Chen, T. Yu, Y. Liu, Y. Sun, M. Lei, N. Guo, Y. Fan, X. Sun, M. Zhang, F. Alarab, V. N. Strocov, Y. Wang, T. Zhou, X. Liu, F. Lu, W. Liu, Y. Xie, R. Peng, H. Xu, and D. Feng, Orientation-dependent electronic structure in interfacial superconductors LaAlO 3/KTaO3, Nature Com...

    2024

  8. [16]

    F. Y. Bruno, S. McKeown Walker, S. Ricc` o, A. de la Torre, Z. Wang, A. Tamai, T. K. Kim, M. Hoesch, M. S. Bahramy, and F. Baumberger, Band Structure and Spin–Orbital Texture of the (111)-KTaO 3 2D Electron Gas, Advanced Electronic Materials5, 1800860 (2019)

    2019

  9. [17]

    J. Yang, C. Liu, X. Zhou, H. Hou, K. Yin, J. Wen, J. Pearson, A. Suslov, D. Jin, J. S. Jiang, U. Welp, J.- M. Zuo, M. R. Norman, and A. Bhattacharya, Uniaxial spin texture in a superconducting electron gas revealed by exchange interactions (2025), arXiv:2502.19599 [cond- mat.supr-con]

    2025 arXiv

  10. [18]

    C. S. B. Pang, B. A. Davidson, F. Li, M. Oudah, P. C. Moen, S. Smit, C. T. Suen, S. Godin, S. A. Gorovikov, M. Zonno, S. Zhdanovich, G. Levy, M. Michiardi, A. M. Hallas, G. A. Sawatzky, R. J. Green, A. Dama- scelli, and K. Zou, Direct fabrication of a superconduct- ing two-dim...

    2025 arXiv

  11. [19]

    For now, we consider the tight binding parameters from the mid- dle column of Table I that we used in our previous work [9, 14] (TB model 1)

    where the chemical potential has been adjusted to give a 2D carrier density ofn 2D = 1014cm−2. For now, we consider the tight binding parameters from the mid- dle column of Table I that we used in our previous work [9, 14] (TB model 1). In Fig. 1a, we show the Fermi surface wi...

  12. [20]

    Z. Chen, A. G. Swartz, H. Yoon, H. Inoue, T. A. Merz, D. Lu, Y. Xie, H. Yuan, Y. Hikita, S. Raghu, and H. Y. Hwang, Carrier density and disorder tuned superconductor-metal transition in a two-dimensional electron system, Nature Communications9, 4008 (2018)

    2018

  13. [21]

    D. Xiao, W. Zhu, Y. Ran, N. Nagaosa, and S. Okamoto, Interface engineering of quantum Hall effects in digital transition metal oxide heterostructures, Nature Commu- nications2, 596 (2011)

    2011

  14. [22]

    A. Jain, S. P. Ong, G. Hautier, W. Chen, W. D. Richards, S. Dacek, S. Cholia, D. Gunter, D. Skinner, G. Ceder, and K. A. Persson, Commentary: The Materials Project: A materials genome approach to accelerating materials innovation, APL Materials1, 011002 (2013)

    2013

  15. [23]

    K. V. Shanavas and S. Satpathy, Electric field tuning of the Rashba effect in the polar perovskite structures, Phys. Rev. Lett.112, 086802 (2014)

    2014

  16. [24]

    K. V. Shanavas, Z. S. Popovi´ c, and S. Satpathy, Theoreti- cal model for Rashba spin-orbit interaction indelectrons, Phys. Rev. B90, 165108 (2014)

    2014

  17. [25]

    M. Kim, J. Ihm, and S. B. Chung, Strongly enhanced Rashba splittings in an oxide heterostructure: A tan- talate monolayer on BaHfO 3, Phys. Rev. B94, 115431 (2016)

    2016

  18. [26]

    W. L. McMillan, Transition temperature of strong- coupled superconductors, Phys. Rev.167, 331 (1968)

    1968

  19. [27]

    Farhi, A

    E. Farhi, A. K. Tagantsev, R. Currat, B. Hehlen, E. Courtens, and L. A. Boatner, Low energy phonon spec- trum and its parameterization in pure KTaO 3 below 80 K, The European Physical Journal B - Condensed Matter and Complex Systems15, 615 (2000)

    2000

  20. [28]

    P. A. Fleury and J. M. Worlock, Electric-field-induced raman scattering in SrTiO3 and KTaO3, Phys. Rev.174, 613 (1968)

    1968

  21. [29]

    Z. Chu, J. Yang, Y. Li, K. Hwangbo, J. Wen, A. R. Bielinski, Q. Zhang, A. B. F. Martinson, S. O. Hruszkewycz, D. D. Fong, X. Xu, M. R. Norman, A. Bhattacharya, and H. Wen, Revealing subterahertz atomic vibrations in quantum para- electrics by surface-sensitive spintronic terah...

    2024 doi

  22. [30]

    van der Marel, F

    D. van der Marel, F. Barantani, and C. W. Rischau, Pos- sible mechanism for superconductivity in doped SrTiO 3, Phys. Rev. Res.1, 013003 (2019)

    2019

  23. [31]

    M. N. Gastiasoro, J. Ruhman, and R. M. Fernandes, Su- perconductivity in dilute SrTiO 3: A review, Annals of Physics417, 168107 (2020)

    2020

  24. [32]

    B. I. Halperin and D. R. Nelson, Resistive transition in superconducting films, Journal of Low Temperature Physics36, 599 (1979)

    1979

  25. [33]

    J. T. Haraldsen, P. W¨ olfle, and A. V. Balatsky, Under- standing the electric-field enhancement of the supercon- ducting transition temperature for complex oxide inter- faces, Phys. Rev. B85, 134501 (2012)

    2012

  26. [34]

    K. Ueno, S. Nakamura, H. Shimotani, A. Ohtomo, N. Kimura, T. Nojima, H. Aoki, Y. Iwasa, and M. Kawasaki, Electric-field-induced superconductivity in an insulator, Nature Materials7, 855 (2008)

    2008

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