# Eta Prime Gluonic Contribution to the Nucleon Self-Energy in an Effective Theory

Authors: A. Upadhyay; J. P. Singh
Journal: Advances in High Energy Physics
 (2014)

---

## Abstract

We estimate a possibleη
′ gluonic contribution to the self-energy of a nucleon in an effective theory. The couplings of the topological charge density to nucleons give rise to OZI violating η
′-nucleon interactions. The one-loop self-energy of nucleon arising due to these interactions is studied using a heavy baryon chiral perturbation theory. The divergences have been removed using appropriate form factors. The nontrivial structure of the QCD vacuum has also been taken into account. The numerical results are sensitive to the choice of the regulator to a nonnegligible extent. We get the total contribution to the nucleon mass coming from its interaction with the topological charge density δ
m
tot
≅
-
(
2.5
–
7.5
)% of the nucleon mass.


---

## Body

## 1. Introduction

The axial anomaly is known to be one of the most subtle effects of the quantum field theory. The axialU
(
1
) symmetry of the QCD Lagrangian is broken by the anomaly. The corresponding pseudoscalar singlet would otherwise have a mass comparable to the pion mass. Such a particle is missing in the spectrum and the lightest candidate would be the η
′ with a mass of 958 MeV, which is considerably heavier than the octet states. Additionally, an important consequence of the axial anomaly is the fact that the would-be Goldstone boson, η
′, is massive even in the chiral limit [1]. The extra mass is induced by nonperturbative gluon dynamics [2–4] and the axial anomaly. In conventional chiral perturbation theory the η
′ is not included explicitly, although it does show up in the form of a contribution to a coupling coefficient of the Lagrangian, a so-called low-energy constant (LEC). Detailed understanding of the proton structure becomes difficult due to the complicated structure of the low-energy QCD.The role of gluonic degrees of freedom and OZI violation in theη
′-nucleon system has been investigated through, among others, the flavor-singlet Goldberger-Treiman relation [5, 6], which, in the chiral limit, reads as
(1)
M
g
A
(
0
)
=
3
2
F
0
(
g
η
′
N
N
-
g
Q
N
N
)
.
Here, g
A
(
0
) is the flavor-singlet axial-charge measured in polarized deep inelastic scattering, g
η
′
N
N is the η
′-nucleon coupling constant, and g
Q
N
N is the one-particle irreducible coupling of the topological charge density Q
=
(
α
s
/
4
π
)
G
G
~ to the nucleon. In (1), M is the nucleon mass and F
0 renormalizes [7, 8] the flavor-singlet decay constant. The coupling constant g
Q
N
N is, in part, related to [5, 6] the amount of spin carried by polarized gluons in a polarized proton. The large mass of η
′ and the small value of g
A
(
0
) = (0.2–0.35), extracted from deep inelastic scattering [9, 10], point to substantial violations of the OZI rule in the flavor-singlet J
P
=
1
+ channel [11]. A large positive g
Q
N
N
~
2.45 is one possible explanation of small value of g
A
(
0
)
|
DIS.It is important to look for significant consequences which are sensitive tog
Q
N
N. OZI violation in the η
′-nucleon system is a probe to the role of the gluons in dynamical chiral symmetry breaking in low-energy QCD. It will be interesting to calculate the nucleon self-energy due to this kind of gluonic interaction. The gluonic contribution to the nucleon self-energy will be over and above the contributions associated with meson exchange models. It is known [12] that the pion self-energy to the nucleon is negative, and it alone contributes (10%–20%) of the nucleon mass. Our objective in this work is to calculate self-energy due to this kind of gluonic interaction.In the conventional chiral perturbation theory, the masses of the ground state baryon octet can be expanded in quark mass as [13] (
m
P
2
~
m
q
)
(2)
M
B
=
M
0
+
∑
q
a
q
m
q
+
∑
q
b
q
m
q
3
/
2
+
∑
q
c
q
m
q
2
+
⋯
.
Borasoy [14] has shown that η
′ can also be included in baryon chiral perturbation theory in a systematic way. In this approach, η
′ is included as a dynamical field variable instead of integrating it out from the effective field theory. It has a justification in 1
/
N
C expansion of QCD [2–4], where the axial anomaly is suppressed by powers of 1
/
N
C and η
′ appears as a ninth Goldstone boson. Since there is no anomaly in the leading order of the 1
/
N
C expansion, it is natural to expect that, up to leading order, the singlet NG boson is present and degenerate with other (
N
f
2
-
1
) nonsinglet NG bosons in the chiral limit. The theory at this level is thus chiral U
(
N
f
)
×
U
(
N
f
) invariant. It is, however, broken by the anomaly which exists in nonleading order of the 1
/
N
C expansion.


## 2. The Low-Energy Effective Lagrangian

Independent of the detailed QCD dynamics, one can construct low-energy effective chiral Lagrangians which include the effect of the anomaly and axialU
(
1
) symmetry and use these Lagrangians to study low-energy processes involving the η and η
′ with OZI violation. In the meson sector, the U
A
(
1
) extended low-energy effective Lagrangian can be written as [15–17]
(3)
L
meson
=
F
π
2
4
Tr
⁡
(
∂
μ
U
∂
μ
U
+
)
+
F
π
2
4
Tr
⁡
[
χ
0
(
U
+
U
+
)
]
+
1
2
i
Q
Tr
⁡
[
log
⁡
U
-
log
⁡
U
+
]
+
3
m
η
0
2
F
0
2
Q
2
,
where U
=
exp
⁡
(
i
(
ϕ
/
F
π
)
+
i
2
/
3
(
η
0
/
F
0
)
) and ϕ
=
∑
k
ϕ
k
λ
k. Here, ϕ
k denotes the octet of would-be Goldstone bosons (π
,
K
,
η
8) arising out of spontaneous breaking of chiral S
U
(
3
)
L
⊗
S
U
(
3
)
R symmetry, η
0 is the singlet boson, and Q is the topological charge density; χ
=
diag
⁡
[
m
π
2
,
m
π
2
,
(
2
m
k
2
-
m
π
2
)
] is the meson mass matrix, the pion decay constant F
π
=
92.4
MeV, and F
0 renormalizes the flavor-singlet decay constant. The U
A
(
1
) gluonic potential involving Q is constructed to reproduce the axial anomaly in the divergence of the renormalized axial-vector current [18]:
(4)
∂
μ
J
μ
5
(
0
)
=
∑
k
=
1
f
2
i
(
m
k
q
k
¯
γ
5
q
k
)
+
N
f
[
α
s
4
π
G
μ
ν
G
~
μ
ν
]
.and to generate the gluonic contribution to theη and η
′ masses.Here,J
μ
5
(
0
)
=
u
¯
γ
μ
γ
5
u
+
d
¯
γ
μ
γ
5
d
+
s
¯
γ
μ
γ
5
s, N
f
=
3, G
μ
ν is the gluon field strength tensor, G
~
μ
ν
=
(
1
/
2
)
ε
μ
ν
α
β
G
α
β, and Q
(
z
)
=
(
α
s
/
4
π
)
G
μ
ν
(
z
)
G
~
μ
ν
(
z
).The low-energy effective LagrangianL
meson is readily extended to include η-nucleon and η
′-nucleon couplings. The chiral Lagrangian for the meson-baryon coupling up to O
(
p
) in the meson momentum is [7, 8]:
(5)
L
mb
=
Tr
⁡
B
¯
(
i
γ
μ
D
μ
-
M
0
)
B
+
F
Tr
⁡
(
B
¯
γ
μ
γ
5
[
a
μ
,
B
]
)
+
D
Tr
⁡
(
B
¯
γ
μ
γ
5
{
a
μ
,
B
}
)
+
i
3
K
Tr
⁡
(
B
¯
γ
μ
γ
5
B
)
Tr
⁡
(
U
+
∂
μ
U
)
-
G
Q
N
N
2
M
0
∂
μ
Q
Tr
⁡
(
B
¯
γ
μ
γ
5
B
)
+
C
F
0
4
Q
2
Tr
⁡
(
B
¯
B
)
.
Here, B represents the baryon octet and M
0 denotes the baryon mass in the chiral limit. D
μ
=
∂
μ
-
i
v
μ is the chiral covariant derivative, v
μ
=
-
(
i
/
2
)
(
ξ
+
∂
μ
ξ
+
ξ
∂
μ
ξ
+
), and a
μ
=
-
(
i
/
2
)
(
ξ
+
∂
μ
ξ
-
ξ
∂
μ
ξ
+
) where ξ
=
U
1
/
2. The S
U
(
3
) couplings are F
=
0.459
±
0
.
008 and D
=
0.798
±
0.008. The axial-vector current has an expansion
(6)
a
u
=
-
1
2
F
π
∂
μ
ϕ
-
1
2
F
0
2
3
∂
μ
η
0
+
⋯
.In continuum QCD, dynamical chiral symmetry breaking is normally studied using Dyson-Schwinger equation for quark and gluon Green’s function [19]. In low-energy effective theories, given by (3) and (5), a flavor independent self-energy of baryon will arise due to interactions of baryons with the topological charge density Q which is flavor- and color-singlet object. This gluonic term Q has no kinetic energy term, but it mixes with η
0 to generate gluonic mass term for η
′. The determination of masses of the physical η and η
′ mesons also requires diagonalization of the (η
8
,
η
0) mass matrix. Thus, part of η mass is also generated by the gluonic term Q [20].The relativistic framework including baryons poses problem due to the existence of a new mass scale, namely, the baryons mass in the chiral limitM
0; a strict chiral counting scheme, that is, a one-to-one correspondence between the meson loops and the chiral expansion, does not exist. In order to overcome this problem, one integrates out the heavy degrees of freedom of the baryons, similar to a Foldy-Wouthuysen transformation, so that a chiral counting scheme emerges. Observables can then be expanded simultaneously in the Goldstone boson octet masses and the η
′ mass that does not vanish in the chiral limit. One obtains a one-to-one correspondence between the meson loops and the expansion in their masses and derivatives both for octet and singlet [14].After integrating out the heavy degrees of freedom of the baryons from the effective theory [21] and assigning a four-velocity v to the baryons, the heavy baryon Lagrangian to the order we are working reads as
(7)
L
mb
=
Tr
⁡
(
B
¯
i
v
·
D
B
)
+
2
F
Tr
⁡
(
B
¯
S
μ
[
a
μ
,
B
]
)
+
2
D
Tr
⁡
(
B
¯
S
μ
{
a
μ
,
B
}
)
+
2
i
3
K
Tr
⁡
(
B
¯
S
μ
B
)
Tr
⁡
(
U
+
∂
μ
U
)
-
G
Q
N
N
M
0
(
∂
μ
Q
)
Tr
⁡
(
B
¯
S
μ
B
)
+
C
F
0
4
Q
2
Tr
⁡
(
B
¯
B
)
,
where S
μ
=
(
i
/
2
)
γ
5
σ
μ
ν
v
ν is the Pauli-Lubanski spin vector.In this work, our objective is to calculate the self-energy of nucleon arising due to gluonic terms within the framework of heavy baryon chiral perturbation theory includingη
′. Heavy baryon chiral perturbation theory is the effective field theory of the standard model at low energies in the baryonic sector which can be successfully applied with Goldstone bosons included. However, traditional S
U
(
3
) heavy baryon chiral perturbation theory does not appear to work well. The leading nonanalytic component from loop corrections destroys the good experimental agreement which exists at lower order. The additional contributions have to be compensated by higher order counter terms. This leads to the problem with convergence of chiral series, and it can be solved using some kind of cutoff regularization instead of common dimensional regularization scheme. Here, dimensionally regularized Feynman diagrams carry implicit and large contributions from short distance physics. In contrast, the cutoff scheme picks out the long distance part of the integral, which behaves, as expected, on physical grounds.Here, we restrict ourselves to the one-loop diagrams of theη and η
′ with the vertices arising due to gluonic interactions with the baryons. For this purpose, we use the following matrix elements [22, 23]:
(8)
〈
0
|
Q
|
η
〉
=
1
3
m
η
2
(
f
8
cos
⁡
θ
-
2
f
0
sin
θ
)
,
〈
0
|
Q
|
η
′
〉
=
1
3
m
η
′
2
(
f
8
sin
θ
+
2
f
0
cos
⁡
θ
)
,
where θ represents the singlet-octet mixing angle parameterized as follows:
(9)
〈
0
|
J
μ
5
(
8
)
|
η
(
p
)
〉
=
2
i
f
8
cos
⁡
θ
p
μ
,
〈
0
|
J
μ
5
(
8
)
|
η
′
(
p
)
〉
=
2
i
f
8
sin
θ
p
μ
,
〈
0
|
J
μ
5
(
0
)
|
η
(
p
)
〉
=
-
6
i
f
0
sin
θ
p
μ
,
〈
0
|
J
μ
5
(
0
)
|
η
′
(
p
)
〉
=
6
f
0
cos
⁡
θ
p
μ
,
J
μ
5
(
8
)
=
1
3
(
u
¯
γ
μ
γ
5
u
+
d
¯
γ
μ
γ
5
d
-
2
s
¯
γ
μ
γ
5
s
)
.
The terms contributing to the mass of the nucleon, δ
m
N, is given in terms of the mass of η and η
′ mesons for monopole, dipole, exponential, and sharp cutoff regularization schemes and is written as follows.For the monopole case,(10)
δ
m
N
=
-
g
Q
N
N
2
m
2
Λ
4
64
π
[
(
2
m
η
+
Λ
(
m
η
+
Λ
)
2
)
m
η
4
M
2
hhhhhhhhhhhh
h
+
(
2
m
η
′
+
Λ
(
m
η
′
+
Λ
)
2
)
m
η
′
4
M
′
2
]
-
ε
Λ
4
16
π
2
F
0
4
[
m
η
4
M
2
Λ
2
-
m
η
2
{
1
+
m
η
2
m
η
2
-
Λ
2
ln
⁡
Λ
2
m
η
2
}
hhhhhhhhhhh
+
m
η
′
4
M
′
2
Λ
2
-
m
η
′
2
{
1
+
m
η
′
2
m
η
′
2
-
Λ
2
ln
⁡
Λ
2
m
η
′
2
}
]
,
for the dipole case,
(11)
δ
m
N
=
-
g
Q
N
N
2
m
2
Λ
4
1
6
2
π
[
m
η
4
M
2
(
Λ
2
(
m
η
+
Λ
)
2
+
Λ
2
m
η
(
m
η
+
Λ
)
4
)
hhhhhhhhhhhhfj
i
+
m
η
′
4
M
′
2
(
Λ
2
(
m
η
′

+

Λ
)
2

+

Λ
2
m
η
′
(
m
η
′

+

Λ
)
4
)
]
-
ε
Λ
4
16
π
2
F
0
4
[
+
m
η
′
4
M
′
2
Λ
2
-
m
η
′
2
{
1
+
m
η
′
2
m
η
′
2
-
Λ
2
ln
⁡
Λ
2
m
η
′
2
}
m
η
4
M
2
Λ
2
-
m
η
2
{
1
+
m
η
2
m
η
2
-
Λ
2
ln
⁡
Λ
2
m
η
2
}
hhhhhhhhhhhh
+
m
η
′
4
M
′
2
Λ
2
-
m
η
′
2
{
1
+
m
η
′
2
m
η
′
2
-
Λ
2
ln
⁡
Λ
2
m
η
′
2
}
]
,
for the exponential case,
(12)
δ
m
N
=
-
g
Q
N
N
2
32
m
2
π
3
/
2
[
×
[
1
-
ϕ
(
m
η
′
Λ
)
]
m
η
4
M
2
(
Λ
3
2
-
Λ
m
η
2
+
π
m
η
3
e
m
η
2
/
Λ
2
)
hhhhhhhhhh
h
×
[
1
-
ϕ
(
m
η
Λ
)
]
+
m
η
′
4
M
′
2
hhhhhhhhhhhhh
⊗
(
Λ
3
2
-
Λ
m
η
′
2
+
π
m
η
′
3
e
m
η
′
2
/
Λ
2
)
h
h
h
h
h
h
h
h
h
h
h
h
h
×
[
1
-
ϕ
(
m
η
′
Λ
)
]
m
η
4
M
2
(
Λ
3
2
-
Λ
m
η
2
+
π
m
η
3
e
m
η
2
/
Λ
2
)
]
-
ε
16
π
2
F
0
4
[
m
η
4
M
2
{
Λ
2
+
m
η
2
e
m
η
2
/
Λ
2
E
i
(
-
m
η
2
Λ
2
)
}
hhhhhhhhhhh
+
m
η
′
4
M
′
2
h
h
h
h
h
h
h
h
h
h
h
h
h
×
{
Λ
2
+
m
η
′
2
e
m
η
′
2
/
Λ
2
E
i
(
-
m
η
′
2
Λ
2
)
}
]
,
and for the sharp cut off case,
(13)
δ
m
N
=
-
g
Q
N
N
2
16
m
2
π
2
[
m
η
4
M
2
(
Λ
3
2
-
Λ
m
η
2
+
m
η
3
ta
n
-
1
Λ
m
η
)
hhhhhhhhhhh
+
m
η
′
4
M
′
2
h
h
h
h
h
h
h
h
h
h
h
h
h
×
(
Λ
3
3
-
Λ
m
η
′
2
+
m
η
′
3
ta
n
-
1
Λ
m
η
′
)
]
-
[
ε
16
π
2
F
0
4
m
η
4
M
2
{
Λ
2
-
m
η
2
ln
⁡
(
Λ
2
+
m
η
2
m
η
2
)
}
h
h
h
h
+
m
η
′
4
M
′
2
{
Λ
2
-
m
η
′
2
ln
⁡
(
Λ
2
+
m
η
′
2
m
η
′
2
)
}
]
,
where
(14)
M
2
=
(
f
8
cos
⁡
θ
-
2
f
0
sin
θ
)
2
6
,
M
′
2
=
(
f
8
sin
θ
-
2
f
0
cos
⁡
θ
)
2
6
.


## 3. Regularization and the Self-Mass

Both the one-loop diagrams given by Figures1(a) and 1(b) are divergent. However, we must remember that we are working in an effective field theory which uses the degrees of freedom and the interactions which are correct only at low energy. It has been shown by Donoghue et al. [13] that any incorrect loop contribution coming from short distance physics can be compensated for by a shift of the parameters of the Lagrangian. Our choice of ultraviolet regulator, which represents a separation scale of long distance physics from the short distance physics, will be dictated by phenomenological considerations. In baryon chiral perturbation theory, which deals with baryons and Goldstone bosons, the separation scale is taken as ~1 fm [13] corresponding to the measured size of a baryon. For our problem, we consider an average “gluonic transverse size” of nucleon [24] 〈
ρ
2
〉
≈
0.24
fm
2 corresponding to a dipole parameterization:
(15)
H
g
(
x
,
t
)
α
(
1
-
t
m
g
2
)
-
2
,
m
g
2
=
1.1
Ge
V
2
,
x
≅
1
0
-
1
.
This gives a two-gluon form factor, which we denote by u, of a nucleon [25] and can be used in the self-energy diagram. Another way to look at this problem is that the U
A
(
1
) gluonic potential involving the topological charge density leads to a contact interaction at a “short distance” (~0.2 fm) where glue is excited in the interaction region [7, 8] of the proton-proton collision and then evolves to become an η or η
′ in the final state. This will lead to a sharp cutoff at an energy scale ~1 GeV.(a) Self-energy diagram and (b) tadpole diagram.
(a)
(b)In the tadpole diagram, we will be usingu, u
2, and u
3
/
2 (geometric mean of the first two), since the phenomenology does not provide any clear cut rule for this. Similarly, three types of form factors will be used in the tadpole diagram for exponential regularization also. Since the use of u in the tadpole diagram does not remove the divergence while u
3
/
2 remains analytic in a restricted region, hence, we use only u
2 for the monopole case. Specifically, our form factor u
(
k
) for monopole, dipole, and exponential regularization has the form, respectively:
(16)
u
(
k
)
=
Λ
2
(
Λ
2
-
k
2
)
,
u
(
k
)
=
Λ
4
(
Λ
2
-
k
2
)
2
,
u
(
k
)
=
exp
⁡
(
k
2
Λ
2
)
.
Dimensional regularization scheme is not particularly suitable for effective field theories since it gets large contributions from short distance physics [13]. We have displayed our numerical results for the self-mass of the nucleon coming from both Figures 1(a) and 1(b), δ
m
N, in Tables 1 and 2. As discussed above, if we consider the regulator mass Λ
≅
1
GeV for the dipole and the sharp cut-off regularization schemes on phenomenological ground, we observe that δ
m
N for dipole (u
3
/
2-column), exponential (u
2-column), and sharp cutoff schemes are approximately same for each mixing angle. Furthermore, δ
m
N for monopole form factor is related to that for exponential form factor (both for u
2-columns) by their regulator scales [12]:
(17)
Λ
exp
⁡
≅
2
Λ
mon
.Table 1
Self-energy of a nucleon,δ
m
N, arising due to its interactions with the topological charge density in monopole, dipole, exponential, and sharp cutoff schemes as a function of regulator scale Λ. η-η
′ mixing angle θ is taken as −18.5°. In dipole and exponential regularizations, in the tadpole diagram the form factor u (which appears at each vertex in the self-energy diagram), u
3
/
2 or u
2, has been used. Numerical values of Λ and δ
m
N are in GeV unit.
Λ (GeV)
δ
m (GeV)
Monopole
Dipole
Exponential
Sharp cutoff
u
u
3
/
2
u
2
u
u
3
/
2
u
2
0.6
−0.033
−0.025
−0.015
−0.004
−0.050
−0.027
−0.017
−0.013
0.8
−0.078
−0.055
−0.036
−0.010
−0.112
−0.062
−0.040
−0.036
1.0
−0.148
−0.100
−0.071
−0.021
−0.206
−0.118
−0.078
−0.076
1.2
−0.248
−0.161
−0.121
−0.037
−0.334
−0.198
−0.135
−0.136Table 2
Self-energy of a nucleon,δ
m
N, in GeV unit, as a function of regulator scale Λ for the same form factors as in Table 1, but for θ
=
-
30.5
°.
Λ (GeV)
δ
m
N (GeV)
Monopole
Dipole
Exponential
Sharp cutoff
u
u
3
/
2
u
2
u
u
3
/
2
u
2
0.6
−0.012
−0.044
−0.006
−0.002
−0.019
−0.011
−0.007
−0.006
0.8
−0.027
−0.088
−0.015
−0.004
−0.042
−0.025
−0.017
−0.016
1.0
−0.049
−0.148
−0.027
−0.009
−0.073
−0.045
−0.032
−0.030
1.2
−0.080
−0.225
−0.044
−0.014
−0.115
−0.073
−0.052
−0.051Hence, we take(18)
δ
m
N
≅
-
0.076
GeV
(
θ
=
-
18.5
°
)
,
≅
-
0.030
GeV
(
θ
=
-
30.5
°
)
.
Self-energy of a nucleon δ
m
N, in dimensional regularization (M
S
¯) scheme, as a function of renormalization point μ, has been calculated for three values of μ
=
0.5, 0.7, and 1.0 GeV for two values of theta and shown in Table 3. η-η
′ mixing angle θ is taken as −18.5° and −30.5° for different regulator scales Λ. If we take the nontrivial structure of the QCD vacuum into account then, in the last term of (7), we can make the replacement Q
2
→
〈
Q
2
〉
+
Q
2
·
〈
Q
2
〉 can be calculated using vacuum saturation hypothesis:
(19)
〈
Q
2
〉
=
(
-
1
384
)
〈
α
s
π
G
2
〉
2
≅
-
(
1
384
)
(
0.012
)
2
Ge
V
8
,
where, for the gluon condensate, we have used the numerical values used by ITEP group [26]. This gives a positive contribution to the nucleon mass:
(20)
δ
m
N
(
0
)
≅
+
0.007
GeV
.Table 3
Self-energy of a nucleon,δ
m
N, in dimensional regularization (M
S
¯) scheme, as a function of renormalization scale µ.
δ
m
N (GeV)
µ (GeV)
θ
=
-
18.5
°
θ
=
-
30.5
°
0.5
−0.260
−0.099
0.7
−0.163
−0.062
1.0
−0.060
−0.023Taking this into account, we get the total contribution to the nucleon mass coming from its interaction with the topological charge density(
δ
m
N
)
tot
≅
-
(
2.5
–
7.5
)
% of the nucleon mass. It is known that the one-loop pion contribution to the nucleon mass is (
δ
m
N
)
pion
≅
-
(
10
–
20
)
% of the nucleon mass [12]. Unlike (
δ
m
N
)
pion, (
δ
m
N
)
tot is flavor independent and is the same for all the members of the octet baryon family. This kind of contribution to baryon mass will not arise in the models with quark-meson interaction only. It is known that the color-magnetic-field energy in the nucleon is negative [27]. Other phenomenological applications, where the precise decoupling mechanism of the massless gluonic mode by the QCD gauge invariance and the nontrivial vacuum structure have been discussed, are in [27–32]. We have not talked about the role of scalar and tensor gluoniums in effective field theories. In particular, scalar gluonium can give rise to Higgs-type mechanism, but this is beyond the scope of the present work.



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