# The Role of Polarons in Cuprates Hi-T

Authors: M. I. Umo
Journal: Indian Journal of Materials Science
 (2014)

---

## Abstract

The phonon contribution to the phenomenon of high temperature superconductivity in the cuprates is argued as being masked as polarons generated by the polarization of the charge reservoir accompanying the Jahn-Teller tilting of the apical oxygen. We discuss the Mahan oscillator-spring extension model as an analogy to the charge reservoir-CuO planec-axis polarons. Using the Boltzmann kinetic equation, we show that the polaron dissociates or collapses at a temperature corresponding to the critical temperature of the superconductor.


---

## Body

## 1. Introduction

Almost three decades since the discovery of high temperature superconductivity in the cuprate La-Ba-CuO by Bednorz and Muller [1] and subsequently in many CuO based compounds by other researchers, there is still no closure about the mechanism of superconductivity in these systems [2, 3]. One of the major points of disagreement is whether phonons contribute along with the accepted spin magnetic fluctuation to the high critical temperature of the cuprates. Many researchers are in support of the phonon mechanism as the only factor responsible for the cuprates high critical temperatures [4–6].Other workers [7–9] have considered the spin magnetic fluctuation the only adoptable theory for the cuprates. A good reason for the persistence of the “phonon-camp,” is perhaps the enduring success of the electron-phonon interaction (EPI) explanation of the low temperature superconductivity (LTS) by Bardeen, Cooper, and Schrieffer (BCS), [10]. Still another reason may be the recent discovery of superconductivity in MgB3 at T
c
=
40 K [11]; this being explained surprisingly by the EPI mechanism. It has even become very comfortable to make prognosis of still higher T
c’s in materials whose electronic properties are well understood based on the EPI. As an example we mention the EPI mechanism used by Gao and his coworkers to predict that the compound Li2B3C superconducts at about 50 K through the process of lifting the σ-bonding up above the Fermi level by doping, enabling σ-electrons to interact strongly with the lattice vibrations in such a way that electron pairing occurs [12]. In the LTS such as lead, tin, and aluminium, phonon contribution is indicated by the isotope effect which relates the critical temperature (T
c) to the mass (M) of the isotope atom as T
c
∝
M
-
α, where α is the electron-phonon coupling constant defined as α
=
-
d
ln
⁡
T
c
/
d
ln
⁡
M. The BCS value for α is 1
/
2 [13] which corresponds to the weak coupling regime where the Coulomb interaction is neglected. When the Coulomb interaction is taken into account, α can be approximated by δ
T
c
/
T
c
=
-
α
(
δ
M
/
M
), where α
=
(
1
/
2
)
[
1
-
(
μ
*
/
(
λ
-
μ
*
)
)
] and λ is the BCS interaction parameter. Thus when the isotope shifts δ
T
c and T
c are known, μ
* the pseudopotential can be defined [14]. The isotope effect also plays a significant role in the cuprates: L
a
2
-
x
S
r
x
Cu
O
4, YBa
2
C
u
3
O
7
-
δ, and N
d
2
-
x
C
e
x
Cu
O
4, where x is the concentration of strontium and cerium, while δ is the oxygen vacancy. Tunneling measurements on these cuprates support a phonon mediated mechanism of superconductivity [15, 16]. Another angle to the phonon contribution to high temperature superconductivity (HTS) is in terms of polarons. A Landau-Pekar-Frohlich polaron is an electronic perturbation of an ionic crystal such that the polarized lattice interacts and moves with the electron as one entity. The first study of the motion of an electron in an ionic crystal was made by Landau [17]. A series of contributions by many researchers have followed since Landau’s work; significantly, by Pekar, Frohlich, and Feynman (for Pekar’s work, see for example, [18–20]). In recent times the EPI mechanism has been reintroduced into condensed matter physics and applied especially to high temperature superconductivity and colossal magnetoresistance by the use of polarons, with some success [5]. A substantive number of papers have addressed the important questions of polaron mass, its radius, ground state energy, and motion [21–24].In the present work we shall study polarons in the cuprates in a somewhat different context. The theory we shall propose here consists of the following. Cooper pairs are preformed even in the pseudogap phase; Jahn-Teller tilting of the apical oxygen in the charge reservoir is responsible for the titration of the CuO plane with electrons or holes. The electrons or holes pairings are created by spin fluctuation scenario [7, 9, 25, 26]. Furthermore, every electron or hole that arrives on the CuO plane is polaronic; the Jahn-Teller tilt causes the polarization whose electrical field is responsible for creating phonons that are exchanged between the polarized ions and the electrons on the CuO plane. The exchange of phonons between the polarized ions and CuO paired electrons constitutes polarons of large radii. Two of such polarons connect the CuO plane of, for example, L
a
2
-
x
S
r
x
Cu
O
4, one from above and another from below. Being massive, the polarons trap and localize the Cooper pair, releasing the pair only at the superconducting transition temperature (T
c).


## 2. Deformation Potential and Lattice Polarization

Consider the positionX
j of a jth atom in an ionic crystal. During lattice vibration the atom is displaced as X
j
=
Q
j
+
u
j, where Q
j is the equilibrium lattice position and u
j is the displacement. Let the motion of X
j be harmonic and described by the Hamiltonian:
(1)
H
o
=
∑
j
(
P
j
2
2
m
+
1
2
m
ω
l
2
u
j
2
)
,
where p
j is the linear momentum, m is the mass, and ω
l is the longitudinal elastic eigen frequency of the atom. In (1) we can substitute the values g
j
=
u
j
m
ω
l and h
j
=
p
j
/
m
ω
l to obtain H
0
=
(
1
/
2
)
ω
l
∑
j
(
h
j
2
+
g
j
2
). We may define the following operators b
j
=
(
1
/
2
)
(
h
j
+
i
g
j
) and b
j
+
=
(
1
/
2
)
(
h
j
-
i
g
j
) which are substituted in H
0 to give the quantum harmonic oscillator Hamiltonian: H
0
=
∑
j
ℏ
ω
l
(
b
j
+
b
j
+
(
1
/
2
)
). From the foregoing results it is easy to show that
(2)
u
j
=
(
1
2
ρ
v
ω
l
)
1
/
2
(
b
j
+
b
j
+
)
.In (2), ρ is the density of the medium, v is the volume, and b
j and b
j
+ are known as the phonon annihilation and creation operators. Since u
j
=
u
j
(
r
), its Fourier transform is
(3)
u
j
=
∑
±
q
u
q
e
i
q
r
=
(
1
2
ρ
v
ω
l
)
1
/
2
∑
q
(
b
q
+
b
-
q
+
)
e
i
q
r
=
(
1
2
ρ
v
ω
l
)
1
/
2
∑
q
(
b
q
e
i
q
r
+
b
q
+
e
-
i
q
r
)
.Let us define the deformation potential as [18]
(4)
𝒰
=
D
I
div
⁡
u
(
r
)
,
where D
I is the deformation constant, and we find
(5)
div
⁡
u
(
r
)
=
∂
∂
r
∑
±
q
u
q
e
i
q
r
=
i
(
1
2
ρ
v
ω
l
)
1
/
2
∑
q
q
(
b
q
e
i
q
r
+
b
q
+
e
-
i
q
r
)
.Thus, the deformation potential becomes(6)
𝒰
=
i
D
I
(
1
2
ρ
v
ω
l
)
1
/
2
∑
q
q
(
b
q
e
i
q
r
+
b
q
+
e
-
i
q
r
)
.The electron can interact with this potential, resulting in the electron-phonon Hamiltonian:(7)
ℋ
ep
=
∫
0
∞
ψ
*
(
r
)
𝒰
ψ
(
r
)
d
3
r
=
D
I
(
1
2
ρ
v
ω
l
)
1
/
2
∑
k
k
′
c
k
+
c
k
′
∑
q
(
b
q
+
b
-
q
+
)
.Here, we chose the limit of integration to reflect a positive direction of electron motion;c
k
=
∑
k
c
k
e
i
k
rand c
k
+
=
∑
k
c
k
+
e
-
i
k
r are the electron annihilation and creation operators, respectively.The polarization of the lattice is defined as(8)
P
→
=
F
∑
q
e
^
q
(
b
q
e
i
q
r
+
b
q
+
e
-
i
q
r
)
,
where e
^
q is the unit vector of polarization and F is the polarization strength which can be determined by writing the polarization in terms of the electric field strength E
→ and normalized atomic deviation ω
→ as
(9)
P
→
=
ω
LO
(
ϵ
0
-
ϵ
∞
4
π
)
1
/
2
ω
→
l
+
ϵ
∞
-
1
4
π
E
→
l
.See [18]. In (9) ϵ
0
,
ϵ
∞ are the static and high frequency dielectric constants, respectively, and ω
LO is the longitudinal optical frequency. The electric field strength is given by E
→
l
=
-
(
ω
LO
/
ϵ
∞
)
(
4
π
(
ϵ
0
-
ϵ
∞
)
)
1
/
2
ω
→
l, ω
→
l is the cut-off longitudinal frequency of the elastic wave related to the transverse frequency ω
t by the Lyddane-Sachs-Teller formula ω
l
/
ω
t
=
(
ϵ
0
/
ϵ
∞
)
1
/
2. When ω
t
=
ω
LO and ω
l
=
(
ϵ
0
/
ϵ
∞
)
1
/
2
ω
LO
=
ω, (9) after a little algebra becomes
(10)
P
→
=
[
ω
l
2
4
π
(
1
ϵ
∞
-
1
ϵ
0
)
]
1
/
2
ω
→
l
=
[
N
μ
ω
l
2
4
π
ϵ
*
]
1
/
2
(
u
→
+
-
u
→
-
)
,
where N is the number of unit cells in unit volume of crystal, μ is the reduced mass of the two ions in the unit cell, and u
→
+, u
→
- are the relative displacements of the positive and negative ions, 1
/
ϵ
*
=
1
/
ϵ
∞
-
1
/
ϵ
0 and ω
→
l
=
(
N
μ
)
1
/
2
(
μ
→
+
-
μ
→
-
). In the continuum approximation
(11)
u
→
+
-
u
→
-
=
(
ρ
v
N
μ
)
1
/
2
∑
q
e
^
j
(
b
q
e
i
q
r
+
b
q
+
e
-
i
q
r
)
.Equation (10) then takes the form
(12)
P
→
=
(
ρ
v
ω
l
2
4
π
ϵ
*
)
1
/
2
e
^
j
∑
q
(
b
q
e
i
q
r
+
b
q
+
e
-
i
q
r
)
.
Equating (8) to (12) we see that F
2
=
(
ρ
ν
ω
l
2
/
4
π
)
(
(
1
/
ϵ
∞
)
-
(
1
/
ϵ
0
)
). Let us now consider the scalar potential ϕ
(
r
) due to the polarization by using the Poisson equation ∇
2
ϕ
=
4
π
div
⁡
P
→; the solution is
(13)
ϕ
(
r
)
=
(
4
π
ρ
v
ω
l
2
ϵ
*
)
1
/
2
(
1
2
ρ
v
ω
l
)
1
/
2
∑
q
1
q
(
b
q
e
i
q
r
+
b
q
+
e
-
i
q
r
)
=
(
2
π
ω
l
e
*
)
1
/
2
∑
q
1
q
(
b
q
e
i
q
r
+
b
q
+
e
-
i
q
r
)
.Then the electron-phonon interaction can also be obtained by using (13) as follows:
(14)
ℋ
ep
=
∫
0
∞
ψ
*
(
r
)
e
ϕ
ψ
(
r
)
d
3
r
=
(
2
π
e
2
ω
l
ϵ
*
)
1
/
2
∑
k
k
′
c
k
+
c
k
′
∑
q
1
q
(
b
q
+
b
-
q
+
)
.Comparing (14) and (7), we obtain a value of the deformation constant D
I as D
I
=
(
4
π
e
2
ω
l
2
ρ
v
/
ϵ
*
)
1
/
2
(
1
/
q
).


## 3. Thec-Axis Polaron

The formation of thec-axis polaron can be described as a spring which is anchored in the deformation potential and stretched to the CuO plane to couple with an electron of the Cooper pair as discussed in Section 1. The polaron then oscillates between these two end points allowing us to study the motion of a harmonic oscillator comprising of longitudinal phonons. The spring motion analogy of the polaron was first used by Feynman [20] and later by Mahan [27] in their works. Within the deformation potential, the ionic system becomes polarized. The polarization wave sets up an electric field E
→
q
=
-
4
π
P
→
q on which electrons scatter; here q denotes the wave vector. Thus
(15)
E
→
q
=
-
4
π
F
∑
q
e
^
j
(
b
q
e
i
q
r
+
b
q
+
e
-
i
q
r
)
.The scalar potentialϕ
(
r
) of the electric field has already been found as (13), and an equivalent expression is obtained by noting that E
→
q
=
-
∇
ϕ
(
r
)
=
-
(
∂
/
∂
r
)
∑
q
ϕ
q
e
i
q
r, so that we can write
(16)
ϕ
(
r
)
=
(
1
2
ρ
v
ω
l
)
1
/
2
∑
q
ϕ
q
e
i
q
r
=
-
(
1
2
ρ
v
ω
l
)
1
/
2
∑
q
4
π
P
q
q
e
i
q
r
=
-
∑
q
4
π
F
q
e
^
q
(
1
2
ρ
v
ω
l
)
1
/
2
(
b
q
e
i
q
r
+
b
q
+
e
-
i
q
r
)
.The potential energy of an electron in this field is thus given as(17)
e
ϕ
=
-
4
π
F
e
(
1
2
ρ
v
ω
l
)
1
/
2
∑
q
1
q
(
b
q
e
i
q
r
+
b
q
+
e
-
i
q
r
)
=
-
(
2
π
e
2
ω
l
e
*
)
1
/
2
∑
q
1
q
(
b
q
e
i
q
r
+
b
q
+
e
-
i
q
r
)
.
Now consider the electron-phonon Hamiltonian (14) which we rewrite in the form
(18)
ℋ
ep
=
(
2
π
e
2
ω
l
ϵ
*
)
1
/
2
ρ
(
k
+
G
)
∑
q
1
q
(
b
q
+
b
-
q
+
)
=
(
2
π
e
2
ω
l
ϵ
*
)
1
/
2
ρ
0
(
k
+
G
)
e
i
G
r
∑
q
1
q
(
b
q
+
b
-
q
+
)
∑
i
e
i
k
r
i
=
∑
q
1
v
1
/
2
(
b
q
+
b
-
q
+
)
∑
i
F
q
(
r
)
e
i
q
r
i
,
where
(19)
F
q
=
∑
G
M
k
+
G
v
1
/
2
ρ
0
(
k
+
G
)
e
i
G
r
∑
q
1
q
and the matrix element of the electron-phonon transition is M
2
=
2
π
e
2
ℏ
ω
l
/
ϵ
*. Now following [27], we write the total Hamiltonian of an electron interacting with the harmonic oscillator as
(20)
ℋ
=
∑
q
{
ω
q
(
b
q
+
b
q
+
1
2
)
+
1
v
1
/
2
(
b
q
+
b
-
q
+
)
∑
i
F
q
(
r
i
)
e
i
q
r
i
}
.The equation of motion technique can be used to find the eigenvalue ofℋ. Indeed for the operator b
q,
(21)
∂
b
q
∂
t
=
i
[
ℋ
,
b
q
]
=
-
i
(
b
q
+
1
v
1
/
2
F
q
ω
q
∑
i
e
i
q
r
i
)
ω
q
.A new operator system can be extracted from (21) as B
q
=
b
q
+
(
(
1
/
v
1
/
2
)
(
F
q
/
ω
q
)
∑
i
e
i
q
r
), B
q
+
=
b
q
+
+
(
(
1
/
v
1
/
2
)
(
F
q
*
/
ω
q
)
∑
i
e
-
i
q
r
i
). These operators satisfy the commutation relations [
B
q
,
B
q
′
+
]
=
δ
q
q
′, [
B
q
,
B
q
′
]
=
[
B
q
+
,
B
q
′
+
]
=
0. Then the Hamiltonian (21) becomes
(22)
ℋ
=
∑
q
ω
q
(
B
q
+
B
q
+
1
2
)
-
1
v
∑
q
|
F
q
|
2
ω
q
|
∑
i
e
i
q
r
i
|
2
with the corresponding eigenvalue being the spring-oscillator system’s energy:
(23)
E
=
∑
q
ω
q
(
N
q
+
1
2
)
-
1
v
∑
q
|
F
q
|
2
ω
q
|
∑
i
e
i
q
r
i
|
2
.The second term of (23) is the relaxation or potential energy of the stretched spring-oscillator, which is justified as follows. Equation (3) can be written as
(24)
u
j
(
t
)
=
(
1
2
ρ
v
ω
l
)
1
/
2
{
B
q
e
-
i
ω
t

+

B
-
q
i
ω
t

-

F
q
v
1
/
2
ω
q
∑
i
e
i
q
r
i
(
e
i
ω
t

+

e
-
i
ω
t
)
}
yielding
(25)
u
j
(
0
)
=
-
2
(
1
2
ρ
v
ω
l
)
1
/
2
∑
q
1
v
1
/
2
F
q
ω
q
∑
i
e
i
q
r
i
.In the Feynman polaron theory, the unit of radius is(
ℏ
/
2
ρ
v
ω
l
)
1
/
2; therefore (25) represents the stretching of the spring-oscillator or polaron by several units. For the sake of completeness of our presentation we shall transform the second term of (23) to show that it is actually the Coulomb potential energy, as
(26)
V
(
r
)
=
-
2
∑
q
F
q
2
ω
l
|
∑
i
e
i
q
r
i
|
2
=
-
2
∑
q
(
e
ϕ
q
)
2
ω
l
|
∑
i
e
i
q
r
|
2
=
-
4
π
e
2
e
*
∫
-
∞
∞
e
i
q
r
q
2
d
3
q
(
2
π
)
3
=
-
1
e
*
(
e
2
r
)
,
where we have put F
q
=
e
ϕ, and volume equal to unity.Physical processes that occur in solids at high temperatures involve large number of phonons. Since the phonon number is never conserved, then it is its average number〈
N
〉 that is relevant. That means 〈
N
〉
=
〈
∑
k
b
k
+
b
k
〉
=
∑
k
∫
ψ
q
*
b
k
+
b
k
ψ
q
d
3
r. One method of carrying out the calculation has been given by Kittel [28], who did the averaging with respect to the first order electron wave function of perturbation theory |
k
,
0
〉
1
=
(
|
k
,
0
〉
+
∑
q
|
k
-
q
,
1
〉
)
〈
k
-
q
,
1
|
H
ep
|
k
,
0
〉
/
(
ε
k
-
ε
k
-
q
-
ω
q
). Thus 〈
N
〉
=
∑
q
(
|
〈
k
-
q
,
1
|
H
ep
|
k
,
0
〉
|
2
/
(
ε
k
-
ε
k
-
q
-
ω
q
)
2
), passing from summation to integration, and after some algebra one obtains the average phonon number in terms of the polaron coupling constant α as |
k
,
0
〉
(27)
〈
N
〉
=
e
2
4
ℏ
ω
l
(
2
m
ω
l
ℏ
)
1
/
2
(
1
ϵ
∞
-
1
ϵ
0
)
=
α
2
,
(28)
α
=
e
2
2
ℏ
ω
l
(
2
m
ω
l
ℏ
)
1
/
2
(
1
ϵ
∞
-
1
ϵ
0
)
.In the case of weak coupling, the self-energy of the polaron can be found by the second order perturbation theory [28]; this calculation will yield as a by-product the polaron effective mass m
p
* in terms of the electron effective mass m
* as
(29)
m
p
*
=
m
*
(
1
+
α
6
)
.Since the polaron potential energy which is the second term of (23) is V
(
r
)
=
-
(
e
2
/
ϵ
*
r
) and the kinetic energy corresponding to the first term is ℏ
ω
(
N
+
(
1
/
2
)
)
=
π
2
ℏ
2
/
2
m
r
2, then the total energy is ℰ
=
(
π
2
ℏ
2
/
2
m
r
2
)
-
(
e
2
/
ϵ
*
r
); minimizing ℰ with respect to r, the explicit form of the polaron radius and minimum energy are seen to be, respectively, [18, 29]:
(30)
r
0
=
π
2
ℏ
2
ϵ
*
m
p
*
e
2
,
ℰ
pol
=
-
m
*
e
4
2
π
2
ℏ
2
ϵ
*
2
=
-
0.051
m
*
e
4
ℏ
2
ϵ
*
2
.


## 4. Polaron Model of Hi-T
c Superconductivity

In this section we shall discuss our polaron model of superconductivity. We shall begin with the diagram of the model as given below in Figure1.Polaronic model: (a) CR refers to the charge reservoir,e
+ is the positive ion obtained after polarization, e
- is one electron of a Cooper pair, points 1 and 1′ and 2 and 2′ are the same points of the sample but are separated by a temperature difference Δ
T
=
T
-
T
c
>
0, ph stands for phonons, and e
* denotes the neutral unpolarized atom. (b) The deformation potential showing the nonequilibrium distribution f at temperature T and the equilibrium distribution f
0 at temperature T
c after relaxation in time τ. The arrow shows the direction of the relaxation. If the charge on the CuO plane is a hole, then the corresponding CR charge is e
-.
(a)
(b)Let us assume that the charges on the CuO plane are the electrons; then the electron-phonon interaction is brought about by the exchange of phonons between the levels 1 and 1′ or statesk and k
′. We denote the probability that phonons make transitions from states k to k
′ in unit time by W
(
k
,
k
′
) and the probability of transitions in the reversed direction by W
(
k
′
,
k
). The Boltzmann transport equation (BTE) can now be introduced in the form
(31)
∂
f
∂
t
=
-
v
∇
r
f
-
1
m
F
∇
v
f
+
∑
k
′
{
W
(
k
,
k
′
)
f
(
k
)
-
W
(
k
′
,
k
)
f
(
k
′
)
}
.Here,f
=
(
e
(
ε
-
ξ
)
/
k
B
T
+
1
)
-
1 is the Fermi-Dirac function, v is the velocity of the electron, r is the position vector, m is the mass, and F is the force on the electron. In the stationary state
(32)
∂
f
∂
t
=
(
∂
f
∂
t
)
field
+
(
∂
f
∂
t
)
col
=
0
.That is,(
∂
f
/
∂
t
)
col
=
-
(
∂
f
/
∂
t
)
field, where the field term is (
∂
f
/
∂
t
)
field
=
-
v
∇
r
f
-
(
1
/
m
)
F
∇
v
f and the collision term is
(33)
(
∂
f
∂
t
)
col
=
∑
k
′
{
W
(
k
,
k
′
)
f
(
k
)
-
W
(
k
′
,
k
)
f
(
k
′
)
}
=
∑
k
′
W
(
k
,
k
′
)
{
f
(
k
)
-
f
(
k
′
)
}
,
where the last equality is due to the principle of detailed balance. In nondegenerate systems, the function f becomes the Boltzmann function, f
(
ε
)
=
e
-
ε
/
k
B
T, thus making the BTE applicable to both electrons and phonons. Let us write (33) in a form conforming to point 1 of Figure 1:
(34)
(
∂
f
∂
t
)
col
(
1
)
=
∑
k
′
W
(
k
,
k
′
)
{
f
(
ε
)

-

f
(
ε
′
)
}

≈

∑
k
′
W
(
k
,
k
′
)
f
(
ε
-
ε
′
)
=
∑
k
′
W
(
k
,
k
′
)
f
(
ω
)
.The points 1 and 2 of Figure1 are related by
(35)
Δ
T
(
∂
f
∂
t
)
col
(
1
)
=
T
c
(
∂
f
∂
t
)
col
(
2
)
and from Figure 1(b) we may form the proportionality relationship f
/
f
0
=
T
0
/
T, so that f
(
ω
)
=
f
0
(
T
0
/
T
1
), where T
c
<
T
0
<
T, and T
1 has been chosen slightly less than T. Then (34) becomes
(36)
(
∂
f
∂
t
)
col
(
1
)
=
∑
k
′
W
(
k
,
k
′
)
f
0
T
0
T
1
and if T
0
≅
T
1, then we can interpret (36) as that uninterrupted phonon transition takes place between the states k and k
′, moderated by the equilibrium distribution function f
0. Now using (35) and (36) we can write for the point 2 of Figure 1, the expression
(37)
(
∂
f
∂
t
)
col
(
2
)
=
-
(
1
-
T
T
c
)
(
∂
f
∂
t
)
col
(
1
)
=
-
∑
k
′
W
(
k
,
k
′
)
f
0
(
1
-
T
T
c
)
.Thus, the collision integral at point 2 is written in terms of the extinction factor1
-
T
/
T
c which indicates the polaron’s collapse at point 2, where T
=
T
c. At T
>
T
c, the polaron energy is greater than the Cooper pair energy 2
Δ. The polaron’s collapse or dissociation is associated with a polaron energy ℰ
pol
=
0 and thus related to the relaxation of the deformation potential in the sense that generally
(38)
(
∂
f
∂
t
)
col
=
-
f
-
f
0
(
ε
)
τ
.That is, when=
f
0
(
ϵ
), the collision integral’s value is given by (37) and point 2 in Figure 1. The value of the matrix elements of the transition probability W
(
k
,
k
′
) has already been found to be
(39)
M
2
=
|
〈
k
′
|
-
e
ϕ
|
k
〉
|
2
=
2
π
e
2
ℏ
ω
l
ϵ
*
.The last expression may directly be obtained by using the Fermi golden rule:(40)
W
(
k
,
k
′
)
=
2
π
ℏ
|
〈
k
′
|
ℋ
e
-
p
|
k
〉
|
2
δ
(
ε
k
-
ε
k
′
∓
ℏ
ω
q
)
.Equation (36) can now be written in the form
(41)
(
∂
f
∂
t
)
col
(
1
)
=
4
π
2
e
2
ω
l
ϵ
*
f
0
T
0
T
1
=
4
π
2
ω
l
α
m
p
*
f
0
T
0
T
1
.The comment made with respect to (36) also holds here.


## 5. Conclusion

For the stability of the polaron system, its energyℰ
pol must be greater than the preformed Cooper pair energy 2
Δ in the temperature regime T
>
T
c. We have assumed that the polarons are localized but oscillating along the c-axis of the cuprate, and when it collapses at T
=
T
c, the Cooper pair which had also been localized becomes free to make translational motion on the CuO plane. This means that for all polaronic superconductors, ℰ
pol
(
T
=
T
c
)
=
0. It is this symbiotic relationship between the polaron and Cooper pair that reveals the mechanism of high temperature superconductivity. Furthermore, based on (37), room temperature superconductivity (see, [30]) can be achieved (at least theoretically) by creating a high temperature polaronic cuprate and searching for T
c in it. The higher the polaron temperature is, the higher the likelihood of finding a room temperature T
c.



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*Source: 590928-2014-03-10.xml*