Article
Logarithmic Correction to the BekensteinHawking Entropy
The Institute of Mathematical Sciences, Chennai 600 113, India.
Physical Review Letters (Impact Factor: 7.51). 03/2000; 84(23). DOI: 10.1103/PhysRevLett.84.5255 Source: arXiv
Fulltext
Available from: Parthasarathi Majumdar, Jan 12, 2013arXiv:grqc/0002040v3 14 Jun 2000
Logarithmic correction to the BekensteinHawking entropy
Romesh K. Kaul and Parthasarathi Majumdar
∗
The Institute of Mathematical Sciences, Chennai 600 113, India.
The exact formula derived by us earlier for the entropy of a four dimensional nonrotating black
hole within the quantum geometry formulation of the event horizon in terms of boundary states of
a three dimensional ChernSimons theory, is reexamined for large horizon areas. In addition to the
semiclassical BekensteinHawking contribution prop ortional to the area obtained earlier, we ﬁnd a
contribution proportional to the logarithm of the area together with subleading corrections that
constitute a series in inverse powers of the area.
The derivation of the BekensteinHawking (BH) area law for black hole entropy from the quantum geometry
approach [1] (and also earlier from string theory [2] for some special cases), has lead to a resurgence of interest in
the quantum aspects of black hole physics in recent times. However, the major activity has remained focusse d on
conﬁrming the area law for large black holes, which, as is wellknown, was obta ined originally on the basis of arguments
of a semiclassical nature. The question arises as to whether any essential feature of the bona ﬁde quantum aspect
of gravity, beyond the do main of the semiclassical approximation, has been captured in these assays. Indeed, as has
been most eloq uently demonstrated by Carlip [3], a derivation of the area law alone seems to be pos sible on the basis
of some symmetry principle of the (semi)classical theory itself without requiring a detailed knowledge of the actual
quantum states associated with a black hole. The result seems to hold fo r arbitrary number of spatial dimensions, so
long as a particular set of isometries of the metric is respected. That quantum gravity has a description in ter ms of
spin networks (or for that matter, in terms of string states in a ﬁxe d background) appears to be of little consequence in
obtaining the area law, although these proposed underlying structures also lead to the same behaviour via alternative
routes, in the semiclassical limit of arbitrarily large horizon area.
Although there is as yet no complete quantum theory of gravitation, one would in general expect key features
uncovered so far to lead to modiﬁcations of the area law which could not have been anticipated through semiclassical
reasoning. Thus, the question as to what is the dominant quantum correction due to these features of quantum gravity
becomes one of pa ramount importance. Already in the string theory literature [4] examples of leading corrections to
the area law, obtained by co unting Dbrane states describing special supers ymmetric extr e mal black holes (interacting
with massless vector supermultiplets) have appeared. This has received strong support recently from semiclassical
calculations in N = 2 supergravity [5] supplemented by ostensible stringy higher derivative corrections which are
incorporated using Wald’s general formalism describing black hole entropy as Noether charge [6]. However, the
geometrical interpretation of these corrections remains unclear. Further, there are s ubtleties associated with direct
application of Wald’s for malism which assumes a nondegenerate bifurcate Killing horizon, to the ca se of extremal
black holes which have degenerate horizons . Moreover, the string results do not pertain to ge neric (i.e., nonextremal)
black holes of Einstein’s general relativity, and ar e constrained by the unphysical requir ement of unbroken spacetime
supe rsymmetry.
In this paper, we cons ider the corrections to the semiclassical area law of generic four dimensional nonrotating
black holes, due to key aspects of nonperturbative quantum gravity (or quantum geometry) formulated by Ashtekar
and c ollaborators [7]. In [1], appropriate boundary conditions are impo sed on dynamical varia bles at the event horizon
considered as an inner boundary. These boundary conditions require that the EinsteinHilbert action be supplemented
by boundary terms describing a thr e e dimensional SU(2) ChernSimons theory living o n a ﬁnite ‘pa tch’ of the horizon
with a spherical boundar y, punctured by links of the spin network bulk states describing the quantum spacetime
geometry interpolating be tween asymptopia and the horizon. On this two dimensional boundary there exists an
SU(2) Wess Zumino model whose conformal blocks describe the Hilbert space of the Cher nSimons theory modelling
the horizon. An exact formula for the number of these conformal blocks has been obtained by us [8] two years ago,
for arbitrary level k and number of punctures p. It has been shown that in the limit of large horizon area given by
arbitrarily large k and p, the logar ithm of this number duly yields the area law. Here we go one step further, and
calculate the dominant subleading contribution, as a function of the classical horizon area, or what is equivalent, as
a function of the BH entropy itself.
On purely dimensional grounds, one would expect the e ntropy to have an expa ns ion, for large classical horizon area,
in inverse powers of area so that the BH term is the leading one,
∗
email: kaul, partha@imsc.ernet.in
1
Page 1
S
bh
= S
BH
+
∞
X
n=0
C
n
A
−n
H
(1)
where, A
H
is the classical horizon area and C
n
are coeﬃcients which are independent of the horizon area but dependent
on the Planck length (Newton constant). Here the Barbero Immirzi parameter [9] has been ‘ﬁtted’ to the value which
ﬁxes the normalization of the BH term to the standard one. However, in principle, one could expect an additional
term proportional to ln A
H
as the leading quantum correction to the semiclassical S
BH
. Such a term is expected on
general grounds pertaining to breakdown of na
¨
ive dimensional analysis due to quantum ﬂuctuations, as is common
in qua ntum ﬁeld theories in ﬂat spacetime and also in quantum theories of critical phenomena. We show, in what
follows, that such a logarithmic correction to the semiclassical area law does indeed arise from the formula derived
earlier [8] and derive its coeﬃcient.
We ﬁrst brieﬂy reca pitulate the derivation [8] of the ge neral formula for the number of conformal blocks of the
SU(2)
k
Wess Zumino model on a punctured 2sphere appropriate to the black hole situation. This number can be
computed in terms of the socalled fusion matrices N
r
ij
[10]
N
P
=
X
{r
i
}
N
r
1
j
1
j
2
N
r
2
r
1
j
3
N
r
3
r
2
j
4
. . . . . . N
j
p
r
p−2
j
p−1
(2)
Diagrammatically, this can be represented as shown in ﬁg. 1 below.
j
p
r
2
r
1
r
p2
j
2
j
3
j
p1
j
1
FIG. 1. Diagrammatic representation of composition of spins j
i
for SU(2)
k
Here, each matrix element N
r
ij
is 1 or 0, depending on whether the prima ry ﬁeld [φ
r
] is allowed or no t in the
conformal ﬁeld theory fusion algebra for the primary ﬁelds [φ
i
] and [φ
j
] (i, j, r = 0, 1/2, 1, ....k/2):
[φ
i
] ⊗ [φ
j
] =
X
r
N
r
ij
[φ
r
] . (3)
Eq. (2) gives the number of conformal blocks with spins j
1
, j
2
, . . . , j
p
on p external lines and spins r
1
, r
2
, . . . , r
p−2
on
the internal lines.
We then use the Verlinde formula [10] to obtain
N
r
ij
=
X
s
S
is
S
js
S
†r
s
S
0s
, (4)
where, the unitary matrix S
ij
diagonalizes the fusion matrix. Upon using the unitarity of the Smatrix, the algebra
(2) reduces to
N
P
=
k/2
X
r=0
S
j
1
r
S
j
2
r
. . . S
j
p
r
(S
0r
)
p−2
. (5)
Now, the matrix elements of S
ij
are known for the case under consideration (SU(2)
k
WessZumino model); they are
given by
S
ij
=
r
2
k + 2
sin
(2i + 1)(2j + 1)π
k + 2
, (6)
where, i, j are the spin labels, i, j = 0, 1/2, 1, ....k/2. Using this Smatrix, the number of conformal blocks for the
set of punctures P is given by
N
P
=
2
k + 2
k/2
X
r=0
Q
p
l=1
sin
(2j
l
+1)(2r+1)π
k+2
h
sin
(2r+1)π
k+2
i
p−2
. (7)
2
Page 2
Eq. (7) thus gives the dimensionality of the SU(2) ChernSimons states corresponding to a thr e e fold bounded by a
twosphere punctured at p points. The black hole microstates are counted by summing N
P
over all sets of punctures
P, N
bh
=
P
{P}
N
P
. Then, the entropy of the black hole is given by S
bh
= log N
bh
.
We are however interested only in the leading correction to the semiclassical entropy which ensues in the limit of
arbitrarily large A
H
. To this end, recall that the eigenvalues of the area opera tor [7] are given by
A
H
= 8πβ l
2
P l
p
X
l=1
[j
l
(j
l
+ 1 )]
1
2
, (8)
where, l
P l
is the P lanck le ngth, j
l
is the spin on the lth puncture on the 2sphere and β is the Barbero Immirzi
parameter [9]. Clearly, the large area limit corresponds to the limits k → ∞ , p → ∞. Now, from eq. (8), it
follows that the number of punctures p is largest for a given A
H
provided all spins j
l
=
1
2
. Thus, for a ﬁxed classical
horizon area, we obta in the la rgest number of punctures p
0
as
p
0
=
A
H
4l
2
P l
β
0
β
, (9)
where, β
0
= 1/π
√
3. In this approximation, the set of punctures P
0
with all spins equal to onehalf dominates over
all other sets, so that the black hole entropy is simply given by
S
bh
= ln N
P
0
, (10)
with N
P
0
being given by eq. (7) with j
l
= 1/ 2.
Observe that N
P
0
can now be written as
N
P
0
=
2
p
0
+2
k + 2
[F (k, p
o
) − F (k, p
0
+ 2 )] (11)
where,
F (k, p) =
[
1
2
(k+1)]
X
ν=1
cos
p
νπ
k + 2
. (12)
The sum over ν in eq. (12) can be approximated by an integral in the limit k → ∞ , p
0
→ ∞, with appropriate
care being taken to restrict the domain of integratio n; one obtains
F (k, p
0
) ≈
k + 2
π
Z
π/2
0
dx cos
p
0
x , (13)
so that,
N
P
0
≈
2
p
0
+2
π(p
0
+ 2 )
B (
p
0
+ 1
2
,
1
2
) , (14)
where, B(x, y) is the standa rd Bfunction [11]. Using wellknown properties of this function, it is straightforward to
show that
ln N
P
0
= p
0
ln2 −
3
2
ln p
0
− ln (2π)
−
5
2
p
−1
0
+ O(p
−2
0
) . (15)
Substituting for p
0
as a function of A
H
from eq. (9) and setting the BarberoImmirzi parameter β to the ‘universal’
value β
0
ln2 [1], one obtains our main result
S
bh
= S
BH
−
3
2
ln
S
BH
ln2
+ const. + ··· , (16)
where, S
BH
= A
H
/4l
2
P l
, and the ellipses denote corrections in inverse powers of A
H
or S
BH
.
3
Page 3
Admittedly, the above calculation is restricted to the leading correction to the semiclassical approximation. It has
been done for a ﬁxed large A
H
by taking the spins on all the punctures to be 1/ 2 so that we have the largest number
of punctures. But it is not diﬃcult to argue that the coeﬃcient of the lnA
H
term is robust in that inclusion of spin
values higher than 1/2 do not aﬀect it, although the c onstant term a nd the coeﬃcients of subleading corrections
with powers of O(A
−1
H
) might get aﬀected. The same appears to be true for values of the level k away from the
asymptotic value which we have ass igned it above: the coeﬃcient of the lnA
H
is once again unaﬀected. Thus, the
leading logarithmic correction with co e ﬃcient 3/2 that we have discerned for the black hole entropy is in this sens e
universal. Moreover, although we have set β = β
0
ln2 in the above formulae, the coeﬃcient of the lnA
H
term is
independent of β, a feature not shared by the s e miclassical area law.
It is therefore clear that the leading correction (and maybe also the subleading ones) to the BH entropy is negative.
One way to understand this could be the informationtheoretic approach of Bekenstein [12]: black hole entropy
represents lack of information about quantum states which arise in the various ways of gravitational collapse that
lead to formation of black holes with the same mass, charge and angular momentum. Thus, the BH entropy is the
‘maximal’ entropy that a black hole can have; incorporation of leading quantum eﬀects reduces the entropy. The
logarithmic nature of the leading correction points to a possible existence of w hat might be called a ‘nonperturbative
ﬁxed point’. That this happens in the physical world of four dimensions is perhaps not without interest.
Recently, the zeroth and ﬁrst law of black hole mechanics have been derived for situations with radiation present
in the vicinity of the horizon, using the notion of the isolated ho rizon [13]. Our conclusions ab ove for the case of
nonrotating black holes hold for such generalizations [1 5 ] as well. Note however that while, the foregoing analysis
involves SU (2)
k
Chern Simons theory, for large k this reduces to a sp e c iﬁc U(1) theory presuma bly related to the
‘gauge ﬁxed’ clas sical theory discussed in [13]. The charge spectrum of this U (1) theor y is discrete and bounded from
above by k. The SU (2) origin of the theory thus provides a natural ‘regularization’ for calculation of the number of
conformal blocks.
Note Added: After the ﬁrst version of this paper appeared in the Archives, it has been brought to our attention
that correc tions to the area law in the form of logarithm of horizon area have been obta ined earlier [14] for extremal
ReissnerNordstrom and dilatonic black holes. These corrections are due to quantum scalar ﬁelds pro pagating in ﬁxed
classical backgrounds appropriate to these black holes. The coeﬃcient of the lnA
H
term that appears in ref. [14] is
diﬀerent from ours. This is only expected, since in contras t to ref. [14], our corrections originate from nonperturbative
quantum ﬂuctuations of spacetime ge ometry (for generic nonrotating black holes), in the absence of matter ﬁelds.
Thus, this correction is ﬁnite and independent of any arbitrary ‘renormalization sc ale’ asso c iated with divergences
due to quantum matter ﬂuctuations in a ﬁxed classical background.
We thank Prof. A. Ashtekar for many illuminating discussions and Prof. R. Mann for useful correspondence.
[1] A. Ashtekar, J. Baez, A. Corichi and K. Krasnov, Phys. Rev. Lett. 80, 904 (1998).
[2] A. Strominger and C. Vafa, Phys. Lett. B379, 99 (1996).
[3] S. Carlip, Class. Quant. Grav. 16, 3327 (1999).
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[5] B. de Wit, Modiﬁcations of the area law and N = 2 supersymmetric black holes, hepth/9906095 and references therein.
[6] R. Wald, Phys. Rev. D48, 3427 (1993); T. Jacobson, G. Kang and R. Myers, Phys. Rev. D49, 6587 (1994); V. Iyer and
R. Wald, Phys. Rev. D50, 846 (1995)..
[7] A. Ashtekar, Lectures on Nonperturbative Canonical Gravity, World Scientiﬁc, 1991; A. Ashtekar and J. Lewandowski in
Knots and Quantum Gravity, ed. J. Baez, Oxford University Press, 1994; Class. Quant. Grav. 14, A55 (1997); J. Baez,
Lett. Math. Phys. 31, 213 (1994); C. Rovelli and L. Smolin, Nucl. Phys. B331, 80 (1990); Nucl. Phys. B442, 593 (1995).
See also references q uoted in A. Ashtekar, Interface of General Relativity, Quantum Physics and St atistical Mechanics:
Some Recent Developments, grqc/9910101.
[8] R. Kaul and P. Majumdar, Phys. Lett. B439, 267 (1998).
[9] F. Barbero, Phys. Rev. D54, 1492 (1996); G. Immirzi, Nucl. Phys. Proc. Suppl. 57, 65 (1997).
[10] P. Di Francesco, P. Mathieu and D. Senechal, Conformal Field Theory, Springer, 1997, p 375.
[11] E. Whittaker and G. Watson, Modern Analysis, Cambridge, 1962.
[12] J. Bekenstein, Phys. Rev. D7, 2333 (1973).
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[14] R. Mann and S. Solodukhin, Nucl. Phys. 523B, 293 (1998) and references therein.
[15] A. Ashtekar, private communication.
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