# A translation invariant bipolaron in the Holstein model and superconductivity

- Victor Lakhno
^{1}Email author

**5**:1277

**DOI: **10.1186/s40064-016-2975-x

© The Author(s) 2016

**Received: **1 July 2016

**Accepted: **1 August 2016

**Published: **8 August 2016

## Abstract

Large-radius translation invariant (TI) bipolarons are considered in a one-dimensional Holstein molecular chain. Criteria of their stability are obtained. The energy of a translation invariant bipolaron is shown to be lower than that of a bipolaron with broken symmetry. The results obtained are applied to the problem of superconductivity in 1D-systems. It is shown that TI-bipolaron mechanism of Bose-Einstein condensation can support superconductivity even for infinite chain.

### Keywords

Delocalized Broken symmetry Strong coupling Canonical transformation Hubbard Hamiltonian Bose condensate## Background

The problem of possible existence of superconductivity in low-dimensional molecular systems has long been of interest to researchers (Williams et al. 1992; Ishiguro et al. 1998; Toyota et al. 2007; Inzelt 2008; Lebed 2008; Altmore and Chang 2013). Presently, it is believed that this phenomenon may occur via a bipolaron mechanism. In three-dimensional systems a bipolaron gas is thought to form a Bose condensate possessing superconducting properties. It is well known that in one-and two-dimensional systems the conditions for bipolarons formation are more favorable than in three-dimensional ones. The main problem in this regard is the fact that in one- and two-dimensional systems Bose-condensation is impossible (Ginzburg 1968).

In papers Tulub (1962), Lakhno (2010, 2012, 2013) and Kashirina et al. (2012) a concept of translation invariant polarons and bipolarons was introduced. Under certain conditions these quasiparticles can possess superconducting properties even if they do not form a Bose condensate. Papers Tulub (1962), Lakhno (2010, 2012, 2013) and Kashirina et al. (2012) dealt with three-dimensional translation-invariant polarons and bipolarons. In the context of the aforesaid it would be interesting to consider the conditions under which translation invariant bipolarons arise in low-dimensional systems. Here the results of Tulub (1962), Lakhno (2010, 2012, 2013) and Kashirina et al. (2012) are applied to the quasi-one-dimensional case corresponding to the Holstein model of a large-radius polaron.

In recent years increased interest in physics of 1D polarons and 1D bipolarons has been considerably provoked by the development of a lot of new materials, such as metal-oxyde ceramics with layered (La\(_2\) (Sr, Br) CuO\(_4\) and (Bi, Tl)\(_2\) (Sr, Ba)\(_2\) CaCuO\(_8\)) or layered-chain (Y Ba\(_2\)Cu\(_3\)O\(_7\)) structure, demonstrating high-temperature superconductivity (Tohyama 2012; Gunnarsson and Rösch 2008; Moriya and Ueda 2000; Benneman and Ketterson 2008), chain organic (polyacetylene) and inorganic ((SN)\(_x\)) polymers, quasi-one-dimensional conducting compounds where charge transfer takes place (TTF TCNQ), etc. (Williams et al. 1992; Ishiguro et al. 1998; Toyota et al. 2007; Inzelt 2008; Lebed 2008; Altmore and Chang 2013; Ginzburg 1968; Tulub 1962; Lakhno 2010, 2012; Kashirina et al. 2012; Lakhno 2013; Tohyama 2012; Gunnarsson and Rösch 2008; Moriya and Ueda 2000; Benneman and Ketterson 2008; Schüttler and Holstein 1986; Emin 1986; Kashirina and Lakhno 2015). Much the same as 1D systems can be materials with huge anisotropy where polarons or bipolarons can emerge (Schüttler and Holstein 1986; Emin 1986; Kashirina and Lakhno 2015). Development of DNA-based nanobioelectronics (Lakhno 2008; Offenhüsser and Rinaldi 2009) is also closely related with calculation of polaron and bipolaron properties in one-dimensional molecular chains (Basko and Conwell 2002; Fialko and Lakhno 2000; Conwell and Rakhmanova 2000; Lakhno and Sultanov 2012). Despite great theoretical efforts, many problems of polaron physics have not been solved yet.

One of the central problems of polaron physics is that of spontaneous breaking of symmetry of the “electron + lattice” system. In most papers on polaron physics, following initial Landau hypothesis (Landau 1933) valid for classical lattice, (see books and reviews Pekar 1963; Kuper and Whitfield 1963; Firsov 1975; Devreese and Peeters 1984; Lakhno 1994; Devreese and Alexandrov 2009; Emin 2013; Kashirina and Lakhno 2013) it is thought that at rather a large coupling an electron deforms a lattice so heavily that it becomes self-trapped in the deformed region. In this case the initial symmetry of the Hamiltonian is broken: an electron passes on from the delocalized state having the Hamiltonian symmetry to the localized “self-trapped” state with broken symmetry. This problem is still more actual for bipolarons since a bipolaron state can arise only in the case of large values of the coupling constant.

As showed in Lakhno (2014) for 1D Holstein polaron in a continuum limit for all the values of the coupling constant, the minimum of its energy in quantum lattice is reached in the class of delocalized wave functions. So in Lakhno (2014) it is shown that in the case of a strong-coupling polaron, symmetry is not broken and a self-trapped state is not formed.

In this paper the results of paper Lakhno (2014) are generalized to the case of 1D bipolaron.

In section “Bipolarons with broken translation invariance in the Holstein model in the strong coupling limit” we present known exact results for a polaron and bipolaron with broken translation invariance in the Holstein continuum model in the strong coupling limit when Coulomb interaction between electrons is lacking. In the general case, when the Coulomb interaction takes place, the properties of the bipolaron ground state are illustrated with the use of a variational approach in which the localized wave function of the exact solution without Coulomb interaction is used as a probe one. The results obtained are used to present the criteria of the bipolaron stability.

In section “Translation invariant bipolaron theory” a translation invariant bipolaron theory is constructed. The wave function of such a bipolaron is delocalized. In the strong coupling limit the functional of the bipolaron total energy is derived.

In section “Variational calculation of the bipolaron state” to study the minimum of the total energy a direct variational method is used. It is shown that, as distinct from a bipolaron with broken symmetry, a translation invariant bipolaron exists for all the values of the Coulomb repulsion constant. The regions where a translation invariant bipolaron is stable relative to its decay into two individual polarons are found. It is shown that for all the values of the Coulomb repulsion parameter, the energy of a translation invariant bipolaron is lower than that of a bipolaron with spontaneously broken symmetry.

In section “Spectrum of excited states” we analyze solutions of the equations for the translation invariant bipolaron (below TI-bipolaron) spectrum. It is shown that the spectrum has a gap separating the ground state of a TI-bipolaron from its excited states which form a quasicontinuous spectrum. The concept of an ideal gas of TI-bipolarons is substantiated.

With the use of the spectrum obtained, in section “Statistical thermodynamics of 1D gas of TI-bipolarons” we consider thermodynamic characteristics of an ideal gas of TI-bipolarons. For various values of the parameters, namely phonon frequencies, we calculate the values of critical temperatures of Bose condensation, latent heat of transition into the condensed state, heat capacity and heat capacity jumps at the point of transition.

In section “Comparison with discrete model” we compare the results for continuum and discrete models.

In section “Discussion of results” we discuss the results obtained.

## Bipolarons with broken translation invariance in the Holstein model in the strong coupling limit

*m*is the electron effective mass, \(\omega ^0_k\) is the frequency of optical phonons,

*g*is the constant of electron-phonon interaction,

*N*is the number of atoms in the chain, \(U(x_1-x_2)\) is the Coulomb repulsion between electrons depending on the difference of electron coordinates which will be taken to be:

In view of an arbitrary position of the bipolaron center of mass \(x_0\), the bipolaron state discussed has an infinite degeneracy and can move along the chain. Any arbitrarily small violation of the chain leads to elimination of the degeneration and localization of the bipolaron state on defects with attracting potential. A qualitatively different situation arises in the case of a translation invariant bipolaron considered below.

## Translation invariant bipolaron theory

*R*in Hamiltonian (2) can be eliminated via Heisenberg canonical transformation Heisenberg (1930):

*r*and, therefore, is automatically translation invariant. It corresponds to the state delocalized over the coordinates of the center of mass of two electrons.

*c*involved in (22) is the same as in Tulub (1962) and Lakhno (2014). In the one-dimensional case under consideration:

## Variational calculation of the bipolaron state

*N*,

*l*,

*a*are variational parameters. As a result, after minimization of (25) on

*N*, the bipolaron energy will be:

*x*,

*y*are presented in Fig. 1 for various values of the parameter \(\gamma\). Figure 1 suggests that as distinct from a bipolaron with broken symmetry [inequality (9)], a translation invariant bipolaron exists for all the values of the parameter \(\gamma\). In the region:

*x*,

*y*involved in (29) are related to the variational parameters

*a*and

*l*(26) and (27) as: \(a=(2ma^2_0g^2/\hbar ^3\omega _0)x, l=(\hbar ^3\omega _0/2ma^2_0g^2)y\). The parameter

*l*determine the characteristic size of the electron pair, i.e. the correlation length \(L(\gamma )\), whose dependence on \(\gamma\) is given by the expression:

The dependencies of \(y_{min}\) and \(x_{min}\) on \(\gamma\) are presented in Fig. 2.

Figure 2 suggests that the correlation length \(L(\gamma )\) in the region of a bipolaron stability \(0<\gamma <\gamma _c\) does not change greatly and for its critical value \(\gamma _c=2.775\) the quantity \(L(\gamma )\) approximately three times exceeds the value of *L*(0), i.e. the correlation length in the absence of the Coulomb repulsion. This qualitatively differs from the case of a bipolaron with broken symmetry for which the corresponding value, according to (6), for \(\gamma =\gamma _c\) turns to infinity.

## Spectrum of excited states

*s*:

Figure 3 suggests that frequencies \(\nu _{k_n}\) occur between the frequencies \(\omega _{k_n}\) and \(\omega _{k_{n+1}}\). Hence, the spectrum of \(\nu _{k_n}\) as well as the spectrum of \(\omega _{k_n}\) is quasi continuous in the continuum limit: \(\nu _{k_n}-\omega _{k_n}=0(N^{-1}_a)\), which proves the validity of (37) and (38).

Therefore the spectrum of a TI-bipolaron has a gap between the ground state of \(E_{bp}\) and the quasi continuum spectrum, which is equal to \(\omega _0\).

Below we will consider the case of low concentration of TI-bipolarons in the chain. In this case they can be adequately considered as Bose-gas, whose properties are determined by Hamiltonian (37).

## Statistical thermodynamics of 1D gas of TI-bipolarons

*N*particles, occurring in a one-dimensional chain of length

*L*. Let us write \(N_0\) for the number of particles in the lower one-particle state, and

*N*for the number of particles in higher states. Then:

Figure 4 suggests that the critical temperature grows as the phonon frequency increases and is equal to zero for \(\omega =0\). The equality \(T_c=0\) for \(\omega =0\) corresponds to the known result, that Bose-condensation is impossible in ideal gas in a one-dimensional case.

Figure 4 also suggests that it is just the increase in the concentration of TI-bipolarons which will lead to an increase in the critical temperature, while the increase in the electron mass *m* to its decrease.

From Fig. 5 it follows that, as we might expect, the number of particles in the condensate grows as the gap \(\omega _i\) increases.

*E*reads:

Relation between \(\tilde{\mu }\) and the chemical potential of the system \(\mu\) is given by the expression \(\tilde{\mu }=(\mu -E_{bp})/\omega ^*\). Formulae (49) and (50) also yield expressions for \(\varOmega\)—potential: \(\varOmega =-2E\) and entropy \(S=-\partial \varOmega /\partial T\) (\(F=-2E, S=-\partial F/\partial T\)).

These dependencies enable us to find the heat capacity of TI-bipolaron gas: \(C_V(\tilde{T})=d\tilde{E}/d\tilde{T}\).

*S*is the entropy of supracondensate particles. At the transition point this value is \(q=2T_cC_V(T_c-0)\),\(C_V=d\tilde{E}/d\tilde{T}\) and \(\tilde{E}\) is determined by formulae (47) and (48). The values of the heat of transition \(q_i\) for the above-cited values of \(\tilde{\omega }_i\) are given in Table 1.

Dependence of critical temperatures \(\tilde{T}_{c_i}\), heat capacities \(C_V(\tilde{T}_{c_i}\pm 0)\), and heat capacity jumps \(\Delta\) on the values of \(\tilde{\omega }_i\)

| 1 | 2 | 3 | 4 | 5 | 6 |

\(\tilde{\omega }_i\) | 0.2 | 1 | 2 | 10 | 15 | 20 |

\(\left. \tilde{T}_{c_i}\right.\) | 5.82 | 14.11 | 20.87 | 53.47 | 68.33 | 81.5 |

\(C_V(\tilde{T}_{c_i}-0)\) | 0.24 | 0.37 | 0.45 | 0.7 | 0.79 | 0.86 |

\(C_V(\tilde{T}_{c_i}+0)\) | 0.17 | 0.23 | 0.25 | 0.32 | 0.33 | 0.34 |

\(\frac{\partial C_V}{\partial \tilde{T}}(\tilde{T}_{c_i}-0)\) | \(5.23\times 10^{-3}\) | \(-0.93\times 10^{-3}\) | \(-2.64\times 10^{-3}\) | \(-4.94\times 10^{-3}\) | \(-5.2\times 10^{-3}\) | \(5.34\times 10^{-3}\) |

\(\frac{\partial C_V}{\partial \tilde{T}}(\tilde{T}_{c_i}+0)\) | \(10.22\times 10^{-3}\) | \(4.72\times 10^{-3}\) | \(3.24\times 10^{-3}\) | \(1.19\times 10^{-3}\) | \(0.89\times 10^{-3}\) | \(0.73\times 10^{-3}\) |

\(\Delta\) | \(5.0\times 10^{-3}\) | \(5.65\times 10^{-3}\) | \(5.88\times 10^{-3}\) | \(6.12\times 10^{-3}\) | \(6.1\times 10^{-3}\) | \(6.06\times 10^{-3}\) |

## Comparison with discrete model

Earlier we considered the problem of symmetry breakdown for one electron interacting with oscillations of a one-dimensional quantum chain (Lakhno 2014). According to Lakhno (2014), a rigorous quantum-mechanical treatment leads to delocalized translation-invariant electron states, or to a lack of soliton-type solutions, breaking the initial symmetry of the Hamiltonian.

In this paper we have shown that when the chain contains two electrons which interact with its oscillations and suffer Coulomb repulsion determined by the interaction, a stable state can be formed which does not violate translation invariance and has a lower energy than the localized solution which breaks TI symmetry does.

*i*,

*j*).

Hamiltonian (1) considered in this work is a continuum analog of Hamiltonian (52) if in (52) we put: \(m=\hbar ^2/2\eta a^2_0, \varGamma =Ua_0\). As is shown in Lakhno (2015b), presentation of the wave function as a product of the electron wave function by the lattice one (Pekar ansatz) does not give an exact solution of Hamiltonian (1). A similar conclusion is valid for Hamiltonian (52). In this context it would be interesting to discuss the limits of applicability of ansatz (53) in a discrete case using a particular example.

*r*is determined by (6). From (6) it also follows that for \(U \ne 0\) Holstein polaron becomes lengthier, since its characteristic size becomes equal to \(r = r_0(1-\gamma /4)^{-1}\), where \(r_0\)—is the characteristic size for \(U=0\). For a TI-bipolaron, the same conclusion follows from expression (33) for the correlation length and Fig. 2. Physically this is explained by the fact that Coulomb repulsion leads to an increase of the characteristic distance between the electrons in the bipolaron state. Earlier this result was also obtained in Emin et al. (1992). Hence, though TI-bipolarons are delocalized, the requirements of continuity for TI-bipolaron and Holstein bipolaron turn out to be similar.

Coupling energies \(\Delta\) for \(U=0\) for a discrete model \(\Delta ^d\), for continuum Holstein model \(\Delta ^H\), and translation invariant bipolaron \(\Delta ^{TI}\)

\(\Delta\) | \(\kappa\) | ||||
---|---|---|---|---|---|

0.1 | 0.1975 | 0.296 | 0.359 | 0.5267 | |

\(\Delta ^d\) | 0.0037 | 0.015 | 0.05 | 0.112 | 0.203 |

\(\Delta ^H\) | 0.0037 | 0.0145 | 0.033 | ||

\(\Delta ^{TI}\) | 0.0056 | 0.022 | 0.0495 |

Table 2 lists the values of \(\Delta\) for which the continuum model is more preferable than the ‘exact’ discrete one.

The results obtained suggest that for parameter values when the continuum model is valid and conditions of strong coupling are met, TI-bipolarons are energetically more advantageous. Therewith the question of the character of a transition from the continuum description to the discrete one remains open. One would expect that such a transition will occur with a sharp increase in the bipolaron effective mass as a result of which the molecular chain will change from highly conducting state to low conducting one.

## Discussion of results

In particular, for \(\gamma = 0\) we get: \(g_c\approx 0.87(\hbar / ma^{2}_{0}\omega _{0})^{1/4}\). Hence, for the overwhelming majority of various systems \(g_c \le 10\).

*H*shifts by \(-g_L \mu _B H/2\), where \(g_L\) is Lande factor, \(\mu _B = |e|\hbar /2mc\) is a Bohr magneton. Being singlet, bipolarons do not experience such a shift. Hence, the region of a bipolaron stability is determined by the inequality \(H < H_c\), where:

As is known, the main mechanism leading to finite resistance in solid bodies is dissipation of charge carriers on phonons Ziman (1960). In the case of translation invariant bipolarons the separation of the system into bipolarons and optical phonons is pointless. For a translation invariant bipolaron in the strong coupling limit, the wave function of the system cannot be divided into electron and phonon parts. The total momentum of a translation invariant bipolaron is a conserving value, the relevant wave function is delocalized over the space and a translation invariant bipolaron occurring in a system consisting only of electrons and phonons, will be superconducting. Inclusion of acoustical phonons into consideration leads to a limitation on the possible value of the velocity *v* of a translation invariant polaron or bipolaron at which they have superconducting properties, namely, according to the laws of energy and momentum conservation, this velocity should be less than that of sound *s*. For \(v > s\), a translation invariant polaron and bipolaron become dissipative.

In a real system containing defects or structural imperfections with attractive potential, these defects and imperfections will always trap polarons and bipolarons with spontaneously broken symmetry. On the contrary translation invariant bipolarons will form a bound state only if the potential well is deep enough. Otherwise, even in an imperfect system, translation invariant bipolarons will be delocalized. Notwithstanding the lack of bound states in the presence of defects, the total momentum of a bipolaron no longer commutates with the Hamiltonian and therefore is not an integral of the system’s motion. In this case a bipolaron will scatter elastically on a defect as a result of which only its momentum will change. This scattering does not lead to an energy loss. In the absence of dissipation the motion of bipolarons will occur without friction and superconductivity in the system will be retained. In the presence of large defects or imperfections possessing a great trapping (scattering) potential, the system under discussion cannot be considered as infinite any longer.

## Conclusions

In this paper we demonstrate that TI-bipolaron mechanism of Bose condensation can support superconductivity even for infinite chain. According to Fig. 6 the condensation in 1D systems is the phase transition of second kind.

The theory resolves the problem of the great value of the bipolaron effective mass. As a consequence, formal limitations on the value of the critical temperature of the transition are eliminated too. The theory quantitatively explains such thermodynamic properties of HTSC-conductors as availability and value of the jump in the heat capacity lacking in the theory of Bose condensation of an ideal gas. The theory also gives an insight into the occurrence of a great ratio between the width of the pseudogap and \(T_c\). It accounts for the small value of the correlation length and explains the availability of a gap and a pseudogap in HTSC materials.

Accordingly, isotopic effect automatically follows from expression (43), where the phonon frequency \(\omega _0\) acts as a gap.

Earlier the 3D TI-bipolaron theory was developed by author in Lakhno (2010, 2012, 2013, 2015b). Consideration of 1D case carried out in the paper can be used to explain 3D high-temperature superconductors (3D TI-bipolaron theory of superconductivity was developed in Lakhno 2015a) where 1D stripes play a great role. As the consideration suggests, artificially created nanostripes with enhanced concentration of charge carriers can be used to increase the critical temperature of superconductors. Theoretical description of the nanostripes can also be based on the approach developed.

## Declarations

### Acknowledgements

The work was supported by projects RFBR N 16-07-00305 and RSF N 16-11-10163.

### Competing interests

The author declares that he has no competing interests.

**Open Access**This article is distributed under the terms of the Creative Commons Attribution 4.0 International License (http://creativecommons.org/licenses/by/4.0/), which permits unrestricted use, distribution, and reproduction in any medium, provided you give appropriate credit to the original author(s) and the source, provide a link to the Creative Commons license, and indicate if changes were made.

## Authors’ Affiliations

## References

- Altmore F, Chang AM (2013) One dimensional superconductivity in nanowires. Wiley, GermanyView ArticleGoogle Scholar
- Basko DM, Conwell EM (2002) Effect of solvation on hole motion in DNA. Phys Rev Lett 88:098102View ArticleGoogle Scholar
- Benneman KH, Ketterson JB (2008) Superconductivity: conventional and unconventional superconductors 1–2. Springer, New YorkView ArticleGoogle Scholar
- Conwell EM, Rakhmanova SV (2000) Polarons in DNA. PNAS 97:4556View ArticleGoogle Scholar
- Devreese JT, Peeters F (eds) (1984) Polarons and excitons in polar semiconductors and ionic crystals. Plenum Press, New YorkGoogle Scholar
- Devreese JT, Alexandrov AS (2009) Fröhlich polaron and bipolaron: recent developments. Rep Prog Phys 72:066501View ArticleGoogle Scholar
- Emin D (1986) Self-trapping in quasi-one-dimensional solids. Phys Rev B 33:3973View ArticleGoogle Scholar
- Emin D, Ye J, Beckel CL (1992) Electron-correlation effects in one-dimensional large-bipolaron formation. Phys Rev B 46:10710View ArticleGoogle Scholar
- Emin D (2013) Polarons. Cambridge University Press, CambridgeGoogle Scholar
- Fialko NS, Lakhno VD (2000) Nonlinear dynamics of excitations in DNA. Phys Lett A 278:108View ArticleGoogle Scholar
- Firsov YA (1975) Polarons. Nauka, MoscowGoogle Scholar
- Ginzburg VL (1968) Problema vysokotemperaturnoy sverhprovodimosti. UFN 95:91View ArticleGoogle Scholar
- Gunnarsson O, Rösch O (2008) Interplay between electronphonon and Coulomb interactions in cuprates. J Phys Condens Matter 20:043201View ArticleGoogle Scholar
- Heisenberg W (1930) Die Selbstenergie des Elektrons. ZS F Phys 65:4View ArticleGoogle Scholar
- Holstein T (1959) Studies of polaron motion: part I. The molecular–crystal model. Ann Phys 8:325View ArticleGoogle Scholar
- Hubbard J (1963) Electron correlations in narrow energy bands. Proc R Soc Lond A 276:238View ArticleGoogle Scholar
- Inzelt G (2008) Conducting polymers. Springer, BerlinGoogle Scholar
- Ishiguro T, Yamaji K, Saito G (1998) Organic superconductors. Springer, BerlinView ArticleGoogle Scholar
- Kashirina NI, Lakhno VD (2010) Large-radius bipolaron and the polaron–polaron interaction. Phys Usp 53:431View ArticleGoogle Scholar
- Kashirina NI, Lakhno VD (2013) Mathematical modeling of autolocalized states in condensed media. Fizmatlit, MoscowGoogle Scholar
- Kashirina NI, Lakhno VD (2014) Continuum model of the one-dimensional Holstein bipolaron in DNA. Math Biol Bioinform 9:430View ArticleGoogle Scholar
- Kashirina NI, Lakhno VD (2015) Bipolaron in anisotropic crystals (arbitrary coupling). Math Biol Bioinform 10:283View ArticleGoogle Scholar
- Kashirina NI, Lakhno VD, Tulub AV (2012) The virial theorem and the ground state problem in polaron theory. JETP 114:867View ArticleGoogle Scholar
- Korepin VE, Eßler FHL (eds) (1994) Exactly solvable models of strongly correlated electrons. Advanced series in mathematical physics, vol 18. World Scientific, SingaporeGoogle Scholar
- Kuper CG, Whitfield GD (eds) (1963) Polarons and excitons. Oliver and Boyd, EdinburghGoogle Scholar
- Lakhno VD (ed) (1994) Polarons and applications. Wiley, ChichesterGoogle Scholar
- Lakhno VD (2006) In: Starikov EB, Lewis JP, Tanaka S (eds) Modern methods for theoretical physical chemistry of biopolymers. Elsevier, AmsterdamGoogle Scholar
- Lakhno VD (2008) DNA nanobioelectronics. Int J Quantum Chem 108:1970View ArticleGoogle Scholar
- Lakhno VD (2010) Energy and critical ionic-bond parameter of a 3D-large radius bipolaron. JETP 110:811View ArticleGoogle Scholar
- Lakhno VD (2012) Translation-invariant bipolarons and the problem of high temperature superconductivity. Solid State Commun 152:621View ArticleGoogle Scholar
- Lakhno VD (2013) Translation invariant theory of polaron (bipolaron) and the problem of quantizing near the classical solution. JETP 116:892View ArticleGoogle Scholar
- Lakhno VD (2014) Large-radius Holstein polaron and the problem of spontaneous symmetry breaking. Prog Theor Exp Phys 2014:073I01View ArticleGoogle Scholar
- Lakhno VD (2015a) TI-bipolaron theory of superconductivity. arXiv:1510.04527 [cond-mat.supr-con]
- Lakhno VD (2015b) Pekar’s ansatz and the strong coupling problem in polaron theory. Phys Usp 58:295View ArticleGoogle Scholar
- Lakhno VD, Sultanov VB (2011) On the possibility of bipolaronic states in DNA. Biophysics 56:210View ArticleGoogle Scholar
- Lakhno VD, Sultanov VB (2012) Possibility of a (bi)polaron high-temperature superconductivity in Poly A/ Poly T DNA duplexes. J Appl Phys 112:064701View ArticleGoogle Scholar
- Landau LD (1933) On the motion of electrons in a crystal lattice. Phys Z Sowjetunion 3:644Google Scholar
- Lebed AG (ed) (2008) The physics of organic superconductors and conductors. Springer series in materials science, vol 110. Springer, Berlin
- Lee TD, Low F, Pines D (1953) The motion of slow electrons in a polar crystal. Phys Rev 90:297View ArticleGoogle Scholar
- Moriya T, Ueda K (2000) Spin fluctuations and high temperature superconductivity. Adv Phys 49:555View ArticleGoogle Scholar
- Offenhüsser A, Rinaldi R (eds) (2009) Nanobioelectronics for electronics, biology, and medicine. Springer, New YorkGoogle Scholar
- Pekar SI (1963) Research in electron theory of crystals (US AEC Transl. AEC-tr-555). United States Atomic Energy Comission. Division of Technical Information, USA, Department of Commerce, Washington; Translated into German: Untersuchungen über die Electronen theorie der Kristalle. Akademie-Verlag, Berlin (1954); Translated from Russian: Issledovaniya po Elektronnoi Teorii Kristallov. GITTL, Moscow-Lenibgrad (1951)
- Proville L, Aubry S (1998) Mobile bipolarons in the adiabatic Holstein–Hubbard model in one and two dimensions. Phys D 113:307View ArticleGoogle Scholar
- Schüttler H-B, Holstein T (1986) Dynamics and transport of a large acoustic polaron in one dimension. Ann Phys 166:93View ArticleGoogle Scholar
- Tohyama T (2012) Recent progress in physics of high-temperature superconductors. Jpn J Appl Phys 51:010004View ArticleGoogle Scholar
- Toyota N, Land M, Müller J (2007) Low dimensional molecular metals. Springer series in solid-state sciences, vol 154. Springer; GmbH & Co., BerlinGoogle Scholar
- Tulub AV (1962) Slow electrons in polar crystals. Sov Phys JETP 14:1301Google Scholar
- Williams JM, Ferraro JR, Torn RJ et al (1992) Organic superconductors: synthesis, structure, properties and theory. Prentice Hall, Englewood CliffsGoogle Scholar
- Ziman JM (1960) Electrons and phonons. Claredon Press, OxfordGoogle Scholar