Einstein-Riemann gravity on deformed spaces
A differential calculus, differential geometry and the E-R Gravity theory are studied on noncommutative spaces. Noncommutativity is formulated in the star product formalism. The basis for the gravity theory is the infinitesimal algebra of diffeomorphisms. Considering the corresponding Hopf algebra w...
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| description | A differential calculus, differential geometry and the E-R Gravity theory are studied on noncommutative spaces. Noncommutativity is formulated in the star product formalism. The basis for the gravity theory is the infinitesimal algebra of diffeomorphisms. Considering the corresponding Hopf algebra we find that the deformed gravity is based on a deformation of the Hopf algebra.
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Symmetry, Integrability and Geometry: Methods and Applications Vol. 2 (2006), Paper 089, 9 pages
Einstein–Riemann Gravity on Deformed Spaces?
Julius WESS †1†2†3
†1 Arnold Sommerfeld Center for Theoretical Physics Universität München,
Theresienstr. 37, 80333 München, Germany
E-mail: wess@theorie.physik.uni-muenchen.de
†2 Max-Planck-Institut für Physik, Föhringer Ring 6, 80805 München, Germany
†3 Universität Hamburg, II Institut für Theoretische Physik and DESY,
Luruper Chaussee 149, 22761 Hamburg, Germany
Received October 27, 2006, in final form November 28, 2006; Published online December 11, 2006
Original article is available at http://www.emis.de/journals/SIGMA/2006/Paper089/
Abstract. A differential calculus, differential geometry and the E-R Gravity theory are
studied on noncommutative spaces. Noncommutativity is formulated in the star product
formalism. The basis for the gravity theory is the infinitesimal algebra of diffeomorphisms.
Considering the corresponding Hopf algebra we find that the deformed gravity is based on
a deformation of the Hopf algebra.
Key words: noncommutative spaces; deformed gravity
2000 Mathematics Subject Classification: 83C65; 81T75; 58B34
This article is based on common work with Paolo Aschieri, Christian Blohmann,
Marija Dimitrijević, Frank Meyer and Peter Schupp [1, 2].
1 Introduction
Gravity theories and differential geometry have been developed on differential manifolds where
the functions form an algebra by pointwise multiplication:
µ{f ⊗ g} = f · g. (1)
In this lecture I want to show that these theories can be generalized by deforming this product.
There are many deformations of the pointwise product to a star product [3, 4, 5, 6]; the simplest
and most discussed is the Moyal–Weyl product [7, 8]:
µ?{f ⊗ g} ≡ f ? g = µ
{
e
ih
2
θρσ∂ρ⊗∂σf ⊗ g
}
, (2)
where θρσ is constant antisymmetric matrix. This product can be shown to be associative but
it is not commutative. It is defined for C∞ functions in general as a formal power series in h.
Evaluated on the functions xµ and xν (1) yields:
xµ ? xν − xν ? xµ ≡ [xµ ?, xν ] = iθµν .
These, mathematically, are the canonical commutation relations of quantum mechanics but here
we postulate them for the configuration space.
?This paper is a contribution to the Proceedings of the O’Raifeartaigh Symposium on Non-Perturbative and
Symmetry Methods in Field Theory (June 22–24, 2006, Budapest, Hungary). The full collection is available at
http://www.emis.de/journals/SIGMA/LOR2006.html
mailto:wess@theorie.physik.uni-muenchen.de
http://www.emis.de/journals/SIGMA/2006/Paper089/
http://www.emis.de/journals/SIGMA/LOR2006.html
2 J. Wess
A differential calculus on noncommutative spaces has been developed [9, 10, 11]. Considering
differentiation as a map from the space of functions to the space of functions:
∂ρ : f 7→ ∂ρf, (3)
it can be generalized to an algebra map.
Recognizing that f ? g is a function, again one finds the deformed Leibniz rule:
∂ρ(f ? g) = (∂ρf) ? g + f ? (∂ρg) + f(∂ρ?)g.
In the case of the Moyal–Weyl product the ? operation is x-independent and we obtain the
usual Leibniz rule. To indicate that the derivative now is a map from the deformed algebra of
functions to the deformed algebra of functions we denote it by ∂?
∂?
ρf ≡ ∂ρf, ∂?
ρ(f ? g) = (∂?
ρf) ? g + f ? (∂?
ρg).
These equations establish a well-defined differential calculus on the deformed space of functions.
They allow us to consider ∂?
ρ as a linear operator with the properties:
∂?
ρ∂
?
σ = ∂?
σ∂
?
ρ (4)
and
∂?
ρf = (∂?
ρf) + f ? ∂?
ρ = (∂ρf) + f ? ∂ρ. (5)
The following treatment of deformed differential geometry will be based on the equations (2),
(4) and (5). It is only the equation (3) that defines the ordinary derivative of a function that
has to be used as an a priori input. The generalization to the deformed situation is essentially
algebraic of nature.
2 Differential operators
We now consider the extension of the algebra of functions (deformed or undeformed) by the
algebra of derivatives. From the Leibniz rule (5) follows that there is a basis where the derivatives
are all at the right hand side of the functions. An element of the extended algebra in this basis
we call a differential operator [1].
Undeformed:
D{d} =
∑
r≥0
dρ1...ρr
r ∂ρ1 · · · ∂ρr .
Deformed:
D?
{d} =
∑
r≥0
dρ1...ρr
r ? ∂?
ρ1
· · · ∂?
ρr
.
A differential operator is characterized by the coefficient functions dr. This is indicated by {d}.
We shall frequently omit this indication and write D for a differential operator, with coefficient
function dr and D′ for d′r.
Differential operators can be multiplied using the algebraic properties (1) or (2) in the de-
formed case and the relations (4) and (5).
The product can always be expressed in terms of differential operators by reordering it with
the help of the Leibniz rule. In this sense the differential operators form an algebra in both
cases, deformed and undeformed.
Einstein–Riemann Gravity on Deformed Spaces 3
There is a map of the operators D to the operators D? that is an algebra morphism
D 7→ D?.
To define this map we let the differential operators act on a function g:
D . g =
∑
r≥0
dρ1...ρr
r
(
∂ρ1 · · · ∂ρrg
)
or D? ?
. g =
∑
r≥0
dρ1...ρr
r ?
(
∂?
ρ1
· · · ∂?
ρr
g
)
.
We now ask for an operator that it, when acting on g, maps g to the same function that we
obtain by acting with the operator D on g. This ?-operator we call X?
D
X?
D
?
. g = D . g. (6)
Because X?
D
?
. g is a function we can apply X?
D̃
once more:
X?
D̃
?
.
(
X?
D . g
)
=
(
X?
D̃ ? X
?
D
)
?
. g.
The left hand side can also be evaluated by using (6) consecutively:
X?
D̃
?
.
(
X?
D
?
. g
)
= X?
D̃
?
.
(
D . g
)
= D̃D . g = X?
D̃D
?
. g.
We conclude:
X?
D̃ ? X
?
D = X?
D̃D. (7)
Multiplying g pointwise with a function f forms a subalgebra of D. We shall now construct
the operator X?
f explicitly for this case starting from (1):
f · g = µ{f ⊗ g} = µ{e
ih
2
θρσ∂ρ⊗∂σe−
ih
2
θρσ∂ρ⊗∂σf ⊗ g} = µ?{e−
ih
2
θρσ∂ρ⊗∂σf ⊗ g}.
More explicitly:
X?
f =
∑
r≥0
1
r!
(
− i
2
)r
θρ1σ1 · · · θρrσr(∂ρ1 · · · ∂ρrf) ? ∂?
σ1
· · · ∂?
σr
.
This operator has the properties:
X?
f ? g = f · g and X?
f ? X
?
g = X?
fg.
Deformed gauge theories [12, 13, 14, 15] are based on these operators.
The algebra of functions with pointwise multiplication is mapped into an algebra of deformed
differential operators.
The algebra of diffeomorphisms is generated by vector fields
ξ = ξµ(x)∂µ,
[ξ, η] =
(
ξµ(∂µη
ρ)− ηµ(∂µξ
ρ)
)
∂ρ = (ξ × η)ρ∂ρ = ξ × η. (8)
The commutator of two vector fields is a vector field again. This is not the case for the star
commutator because the ?-product of two functions does not commute. The differential opera-
tors X?
ξ , however, will form an algebra under the star commutator:
[X?
ξ
?, X?
η ] = X?
ξ×η.
This follows from (7).
4 J. Wess
The operator X?
ξ is easily constructed starting from (2)
ξ . g = ξµ∂µ . g = ξµ(∂µg) = X?
ξµ ? ∂?
µ
?
. g.
Thus, we find
X?
ξ = X?
ξµ ? ∂?
µ.
Again the usual algebra of diffeomorphisms is mapped into a subalgebra of the algebra D?
ξ 7→ X?
ξ , [X?
ξ
?, X?
η ] = X?
ξ×η.
This is the starting point for the construction of a tensor calculus on tensor fields.
3 Tensor fields
The classical theory of gravity is based on invariance under coordinate transformations. This
leads to the concept of scalar, vector and tensor fields that transform under general coordinate
transformation as follows
scalar: δξφ(x) = −ξφ,
covariant vector: δξVµ(x) = −ξVµ − (∂µξ
ρ)Vρ,
contravariant vector: δξV
µ(x) = −ξV µ + (∂ρξ
µ)V ρ
and so on.
The concept of coordinate transformations is difficult to generalize to deformed spaces, but
the transformation laws of fields are representations of the infinitesimal diffeomorphism algebra
that we know how to deform. Thus, we will postulate the following transformation laws for the
deformed algebra of diffeomorphisms
δ?
ξφ(x) = −X?
ξ
?
. φ,
δ?
ξVµ(x) = −X?
ξ
?
. Vµ −X?
(∂µξρ)
?
. Vρ,
δ?
ξV
µ(x) = −X?
ξ
?
. V µ +X?
(∂ρξµ)
?
. V ρ
and so on.
To construct Lagrangians we have to know how the ?-product of fields transforms. These
products should transform as tensor fields again. E.g., the ?-product of two scalar fields should
transform as a scalar field again
δ?
ξ (φ ? ψ) = −X?
ξ
?
. (φ ? ψ). (9)
A lengthy but direct calculation shows that this is identical to:
δ?
ξ (φ ? ψ) = −µ?{F∆(ξ)F−1φ⊗ ψ}, (10)
where ∆(ξ) is the usual comultiplication
∆(ξ) = ξ ⊗ 1 + 1⊗ ξ
and therefore an element of the ⊗ tensor product. F is called a twist and it is an element of the
tensor product
F = e−
ih
2
θρσ∂ρ⊗∂σ . (11)
Einstein–Riemann Gravity on Deformed Spaces 5
The right hand side of (9) and (10) can be calculated in a power series expansion in h and will
be found to be the same.
The advantage of the expression (10) is that it links to the formalism of deforming Hopf
algebras by twists [16, 17, 18, 19]. Many results are known there. We first have to establish
that F really satisfies the conditions for a twist [2]. For (11) it is the case. Then we can use the
twist to deform the Leibniz rule for arbitrary tensor fields. The procedure is as follows:
First consider the coproduct for the undeformed transformations
∆(δξ) = δξ ⊗ 1 + 1⊗ δξ,
where the variations δξ are expressed by differential operators such that
δξ(φ⊗ ψ) = (δξφ)⊗ ψ + φ⊗ (δξψ)
for any two tensor fields φ and ψ. This coproduct can be twisted
∆F (δξ) = F∆(δξ)F−1.
Finally the Leibniz rule becomes
δ?
ξ (φ ? ψ) = µ?{∆F (δξ)φ⊗ ψ}. (12)
This is not limited to scalar fields but covers the ?-product of all tensor fields.
Finally we can convince ourselves that this Leibniz rule has the properties demanded at the
beginning of this chapter, i.e. that ?-products of tensor fields transform as tensor fields.
Equation (12) allows us now to consider ?-products of fields and to determine their transfor-
mation properties.
As a Hopf algebra the algebra of infinitesimal diffeomorphisms is deformed!
4 Einstein–Hilbert gravity
The Einstein–Hilbert theory of gravity can now be constructed following its presentation in a
text book.
4.1 Covariant derivatives
The covariant derivative of a tensor field should again transform as a tensor field. This can be
done with the help of a connection Γ. For a covariant vector field:
Dµ
?
. Vν = ∂?
µ
?
. Vν − Γα
µν ? Vα.
To be a covariant derivative the connection has to transform as follows:
δ?
ξΓ
α
µν = −X?
ξ
?
. Γα
µν −X?
(∂µξρ)
?
. Γα
ρν −X?
(∂νξρ)
?
. Γα
µρ +X?
(∂ρξα)
?
. Γρ
µν − ∂µ∂νξ
α. (13)
This can easily be generalized to arbitrary tensor fields.
4.2 Curvature and torsion
The curvature and torsion tensors can be defined as usual
[Dµ
?, Dν ] ? Vρ = Rµνρ
σ ? Vσ + Tµν
α ? DαVρ.
They can be expressed in terms of the connection:
Rµνρ
σ = ∂?
ν
?
. Γσ
µρ − ∂?
µ
?
. Γσ
νρ + Γβ
νρ ? Γσ
µβ − Γβ
µρ ? Γσ
νβ, (14)
Tµν
α = Γα
νµ − Γα
µν .
From the transformation law of the connection (13) follows that curvature and tension transform
like tensors if the deformed Leibniz rule (12) is used.
6 J. Wess
4.3 Metric tensor
The relevant dynamical variable in gravity is the metric tensor. It is introduced as a covariant
symmetric tensor of rank two:
δ?
ξGµν = −X?
ξ
?
. Gµν −X?
(∂µξρ)
?
. Gρν −X?
(∂νξρ)
?
. Gµρ. (15)
For θ = 0 we identify it with the usual metric field:
Gµν
∣∣∣
θ=0
= gµν . (16)
We will see that gµν is the only dynamical variable in the Einstein–Hilbert theory.
Next we have to construct the ?-inverse of the metric:
Gµν ? G
νρ? = δρ
µ.
Let us first construct the ?-inverse of a function that is invertible in the undeformed algebra:
f · f−1 = 1.
The star inverse f−1? is defined by
f ? f−1? = 1.
It exists as a geometric series because f−1 exists. The additional terms are a power series in θ.
To find f−1? in a compact version we start from
f ? f−1 = 1 +O(θ),(
f ? f−1
)−1? =
(
1 + f ? f−1 − 1
)−1? =
∞∑
n=0
(
1− f ? f−1
)n?
. (17)
The star at the nth power means that all the products are star products. By definition we know
that
(f ? f−1) ? (f ? f−1)−1? = 1. (18)
The star multiplication is associative. We use this for equation (18) and write it in the form
f ?
(
f−1 ? (f ? f−1)−1?
)
= 1.
It follows that
f−1? = f−1 ? (f ? f−1)−1?. (19)
The factor (f ? f−1)−1? has been calculated in (17) as a power series expansion in f and f−1.
We insert this into (19) and find that f−1? can be expressed in f and f−1.
To invert the metric tensor we follow the analogous procedure.
Gµν ·Gνρ = δρ
µ, Gµν ? G
νρ? = δρ
µ
are the defining equations for Gµν and Gµν?. For Gµν? we find
Gµν? = Gµρ ? (G ? G−1)−1? ν
ρ , (20)
Einstein–Riemann Gravity on Deformed Spaces 7
where G and G−1 are short for the matrices Gµν and Gµν respectively. We also can show that
(G ? G−1)−1? =
∑
n≥0
(
1−G ? G−1
)n?
.
Because the ?-product is not commutative Gµν? will be not symmetric in µ and ν. Note that we
always work with the formal power series expansions (in the sense that they do not necessarily
converge), so the solutions for the inverses (19) and (20) are formal.
It can now be shown explicitly from the transformation law (15) for Gµν that Gµν? transforms
as a contravariant tensor of rank 2. Deformed Leibniz rule!
In formulating the ER theory we meet the determinant and the square root of the determinant.
As it is more difficult to generalize the square root to a ?-square root we first introduce the
vielbein as the “square” root of the metric tensor. It consists of four covariant vector fields E a
µ
that form the metric:
Gµν = 1
2
(
E a
µ ? E b
ν + E a
ν ? E b
µ
)
ηab.
As the ?-product is noncommutative we have symmetrized Gµν explicitly. For the vielbein fields
we demand in analogy with (16)
E a
µ
∣∣∣
θ=0
= e a
µ .
From the vector-like transformation properties of E a
µ follows that Gµν transforms like a tensor.
The determinant of the vielbein is defined as follows:
E? = det?E
a
µ = 1
4!ε
µ1...µ4εa1...a4E
a1
µ1
? · · · ? E a4
µ4
. (21)
The star on E? and det? indicates that all the multiplications are ?-multiplications. This nor-
malization was chosen such that
det?E
a
µ
∣∣∣
θ=0
= dete a
µ .
The second ε-tensor is necessary because the ?-product is noncommutative.
The important property of the determinant is that it transforms as a scalar density:
δ?
ξE
? = −X?
ξ
?
. E? −X?
(∂µξµ)
?
. E?. (22)
This is a consequence of the transformation law of the vielbein. This justifies the definition (21)
of the determinant.
We now have all the ingredients we need to proceed for the formulation of the Einstein–Hilbert
dynamics.
4.4 Christoffel symbol
We demand that the covariant derivative of Gµν vanishes:
DαGβγ = ∂?
α
?
. Gβγ − Γρ
αβ ? Gργ − Γρ
αγ ? Gβρ = 0.
We permute the indices, assume that Gαβ is symmetric and obtain by following the analogous
procedure in the classical case:
Γσ
αβ = 1
2
(
∂?
α
?
. Gβγ + ∂?
β
?
. Gαγ − ∂?
γ
?
. Gαβ
)
? Gγσ?.
The connection is entirely expressed in terms of Gαβ . In this case we call the connection
Christoffel symbol.
Again the transformation law of the connection (13) follows from the transformation law
of Gαβ .
8 J. Wess
4.5 Ricci tensor and curvature scalar
We obtain the Ricci tensor by contracting the upper index with one of the three lower indices
of the curvature tensor (14). As the curvature tensor is antisymmetric in the first two indices
we have only two choices left. Contracting of the second index is a deformation of the classical
Ricci tensor:
Rµν = Rµσν
σ. (23)
The contraction Rµνσ
σ vanishes in the classical limit θ → 0. Nevertheless, we could add such
a term to the Ricci tensor (23) and obtain a deformation of the classical Ricci tensor.
We see that the deformation of the classical theory is not unique. Terms that are covariant
and vanish for θ → 0 are quite possible. To really make the deformation unique an additional
requirement has to be added. We take simplicity and define the Ricci tensor by (23).
The curvature scalar we define by contraction with Gµν?
R = Gµν? ? Rµν .
Again, as Gµν? is not symmetric this is a choice.
We can now show by starting from the tensor Gµν that the curvature scalar transforms as
a scalar field
δ?
ξR = −X?
ξ
?
. R = −ξµ(∂µR). (24)
4.6 Lagrangian
The curvature scalar multiplied by the determinant E? transforms like a scalar density. From (24)
and (22) follows:
δ?
ξ (E
? ? R) = −∂?
µ
?
.
(
X?
ξµ
?
. (E? ? R)
)
.
To define an action and the variational principle to find the field equation we have to give
a definition for the integral. A possible definition is∫
f =
∫
d4x f. (25)
This integral has the trace property∫
d4x f ? g =
∫
d4x g ? f.
A suitable action for a gravity theory on deformed spaces is:
SEH =
1
2
∫
d4x
(
E? ? R+ c.c.
)
.
A reminder: By all the transformation laws of products of fields the deformed Leibniz rule (12)
has to be used.
4.7 Field equations
The trace property of the integral (25) allows us to define a variational principle. Vary one field
after the other but always bring it first to the left (right) hand side of the integral by using the
trace property.
Einstein–Riemann Gravity on Deformed Spaces 9
[1] Aschieri P., Blohmann C., Dimitrijević M., Meyer F., Schupp P., Wess J., A gravity theory on noncommu-
tative spaces, Classical Quantum Gravity, 2005, V.22, 3511–3522, hep-th/0504183.
[2] Aschieri P., Dimitrijević M., Meyer F., Wess J., Noncommutative geometry and gravity, Classical Quantum
Gravity, 2006, V.23, 1883–1912, hep-th/0510059.
[3] Bayen F., Flato M., Fronsdal C., Lichnerowicz A., Sternheimer D., Deformation theory and quantization. I.
Deformations of symplectic structures, Ann. Physics, 1978, V.111, 61–110.
[4] Sternheimer D., Deformation quantization: twenty years after, AIP Conf. Proc., 1998, V.453, 107–145,
math.QA/9809056.
[5] Kontsevich M., Deformation quantization of Poisson manifolds, Lett. Math. Phys., 2003, V.66, 157–216,
q-alg/9709040.
[6] Waldman S., An introduction to deformation quantization, Lecture Notes, 2002,
see http://idefix.physik.uni-freiburg.de/∼stefan/Skripte/intro/index.html.
[7] Weyl H., Quantenmechanik und Gruppentheorie, Zeit. für Phys., 1927, V.46, 1–46.
[8] Moyal J.E., Quantum mechanics as a statistical theory, Proc. Cambridge Phil. Soc., 1949, V.45, 99–124.
[9] Wess J., Zumino B., Covariant differential calculus on the quantum hyperplane, Nuclear Phys. B Proc.
Suppl., 1991, V.18, 302–312.
[10] Woronowic S.L., Differential calculus on compact matrix pseudogroups (quantum groups), Comm. Math.
Phys., 1989, V.122, 125–170.
[11] Wess J., Deformed coordinate spaces; derivatives, in Proceedings of the BW2003 Workshop on Mathema-
tical, Theoretical and Phenomenological Challenges Beyond the Standard Model: Perspectives of Balkans
Collaboration (2003, Vrnjačka Banja, Serbia), Vrnjačka Banja, 2003, 122–128, hep-th/0408080.
[12] Wess J., Differential calculus and gauge transformations on a deformed space, hep-th/0607251.
[13] Wess J., Deformed gauge theories, hep-th/0608135.
[14] Aschieri P., Dimitrijević M., Meyer F., Schraml S., Wess J., Twisted gauge theories, Lett. Math. Phys., 2006,
V.78, 61–71, hep-th/0603024.
[15] Vassilevich D.V., Twist to close, Modern Phys. Lett. A, 2006, V.21, 1279–1284, hep-th/0602185.
[16] Drinfel’d V.G., On constant quasiclassical solutions of the Yang–Baxter equations, Soviet Math. Dokl., 1983,
V.28, 667–671.
[17] Reshetikhin N., Multiparameter quantum groups and twisted quasitriangular Hopf algebras, Lett. Math.
Phys., 1990, V.20, 331–335.
[18] Gerstenhaber M., Giaquinto A., Schack S.D., Quantum symmetry, in Quantum Groups, Lecture Notes in
Math., V.1510, Editor P.P. Kulish, Berlin, Springer-Verlag, 1992, 9–46.
[19] Kulish P.P., Lyakhovsky V.D., del Olmo M.A., Chains of twists for classical Lie algebras, J. Phys. A: Math.
Phys., 1999, V.32, 8671–8684, math.QA/9908061.
http://arxiv.org/abs/hep-th/0504183
http://arxiv.org/abs/hep-th/0510059
http://arxiv.org/abs/math.QA/9809056
http://arxiv.org/abs/q-alg/9709040
http://idefix.physik.uni-freiburg.de/~stefan/Skripte/intro/index.html
http://arxiv.org/abs/hep-th/0408080
http://arxiv.org/abs/hep-th/0607251
http://arxiv.org/abs/hep-th/0608135
http://arxiv.org/abs/hep-th/0603024
http://arxiv.org/abs/hep-th/0602185
http://arxiv.org/abs/math.QA/9908061
1 Introduction
2 Differential operators
3 Tensor fields
4 Einstein-Hilbert gravity
4.1 Covariant derivatives
4.2 Curvature and torsion
4.3 Metric tensor
4.4 Christoffel symbol
4.5 Ricci tensor and curvature scalar
4.6 Lagrangian
4.7 Field equations
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| id | nasplib_isofts_kiev_ua-123456789-146064 |
| institution | Digital Library of Periodicals of National Academy of Sciences of Ukraine |
| issn | 1815-0659 |
| language | English |
| last_indexed | 2025-12-07T18:37:24Z |
| publishDate | 2006 |
| publisher | Інститут математики НАН України |
| record_format | dspace |
| spelling | Wess, J. 2019-02-06T17:15:35Z 2019-02-06T17:15:35Z 2006 Einstein-Riemann gravity on deformed spaces / J. Wess // Symmetry, Integrability and Geometry: Methods and Applications. — 2006. — Т. 2. — Бібліогр.: 19 назв. — англ. 1815-0659 2000 Mathematics Subject Classification: 83C65; 81T75; 58B34 https://nasplib.isofts.kiev.ua/handle/123456789/146064 A differential calculus, differential geometry and the E-R Gravity theory are studied on noncommutative spaces. Noncommutativity is formulated in the star product formalism. The basis for the gravity theory is the infinitesimal algebra of diffeomorphisms. Considering the corresponding Hopf algebra we find that the deformed gravity is based on a deformation of the Hopf algebra. This paper is a contribution to the Proceedings of the O’Raifeartaigh Symposium on Non-Perturbative and
 Symmetry Methods in Field Theory (June 22–24, 2006, Budapest, Hungary). en Інститут математики НАН України Symmetry, Integrability and Geometry: Methods and Applications Einstein-Riemann gravity on deformed spaces Article published earlier |
| spellingShingle | Einstein-Riemann gravity on deformed spaces Wess, J. |
| title | Einstein-Riemann gravity on deformed spaces |
| title_full | Einstein-Riemann gravity on deformed spaces |
| title_fullStr | Einstein-Riemann gravity on deformed spaces |
| title_full_unstemmed | Einstein-Riemann gravity on deformed spaces |
| title_short | Einstein-Riemann gravity on deformed spaces |
| title_sort | einstein-riemann gravity on deformed spaces |
| url | https://nasplib.isofts.kiev.ua/handle/123456789/146064 |
| work_keys_str_mv | AT wessj einsteinriemanngravityondeformedspaces |