# Gravitational instanton

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In mathematical physics and differential geometry, a gravitational instanton is a four-dimensional complete Riemannian manifold satisfying the vacuum Einstein equations. They are so named because they are analogues in quantum theories of gravity of instantons in Yang–Mills theory. In accordance with this analogy with self-dual Yang–Mills instantons, gravitational instantons are usually assumed to look like four dimensional Euclidean space at large distances, and to have a self-dual Riemann tensor. Mathematically, this means that they are asymptotically locally Euclidean (or perhaps asymptotically locally flat) hyperkähler 4-manifolds, and in this sense, they are special examples of Einstein manifolds. From a physical point of view, a gravitational instanton is a non-singular solution of the vacuum Einstein equations with positive-definite, as opposed to Lorentzian, metric.

There are many possible generalizations of the original conception of a gravitational instanton: for example one can allow gravitational instantons to have a nonzero cosmological constant or a Riemann tensor which is not self-dual. One can also relax the boundary condition that the metric is asymptotically Euclidean.

There are many methods for constructing gravitational instantons, including the Gibbons–Hawking Ansatz, twistor theory, and the hyperkähler quotient construction.

## Taxonomy

By specifying the 'boundary conditions', i.e. the asymptotics of the metric 'at infinity' on a noncompact Riemannian manifold, gravitational instantons are divided into a few classes, such as asymptotically locally Euclidean spaces (ALE spaces), asymptotically locally flat spaces (ALF spaces). There also exist ALG spaces whose name is chosen by induction.

## Examples

It will be convenient to write the gravitational instanton solutions below using left-invariant 1-forms on the three-sphere S3 (viewed as the group Sp(1) or SU(2)). These can be defined in terms of Euler angles by

${\displaystyle \sigma _{1}=\sin \psi \,d\theta -\cos \psi \sin \theta \,d\phi }$
${\displaystyle \sigma _{2}=\cos \psi \,d\theta +\sin \psi \sin \theta \,d\phi }$
${\displaystyle \sigma _{3}=d\psi +\cos \theta \,d\phi .}$

### Taub–NUT metric

${\displaystyle ds^{2}={\frac {1}{4}}{\frac {r+n}{r-n}}dr^{2}+{\frac {r-n}{r+n}}n^{2}{\sigma _{3}}^{2}+{\frac {1}{4}}(r^{2}-n^{2})({\sigma _{1}}^{2}+{\sigma _{2}}^{2})}$

### Eguchi–Hanson metric

The Eguchi–Hanson space is important in many other contexts of geometry and theoretical physics. Its metric is given by

${\displaystyle ds^{2}=\left(1-{\frac {a}{r^{4}}}\right)^{-1}dr^{2}+{\frac {r^{2}}{4}}\left(1-{\frac {a}{r^{4}}}\right){\sigma _{3}}^{2}+{\frac {r^{2}}{4}}(\sigma _{1}^{2}+\sigma _{2}^{2}).}$

where ${\displaystyle r\geq a^{1/4}}$. This metric is smooth everywhere if it has no conical singularity at ${\displaystyle r\rightarrow a^{1/4}}$, ${\displaystyle \theta =0,\pi }$. For ${\displaystyle a=0}$ this happens if ${\displaystyle \psi }$ has a period of ${\displaystyle 4\pi }$, which gives a flat metric on R4; However, for ${\displaystyle a\neq 0}$ this happens if ${\displaystyle \psi }$ has a period of ${\displaystyle 2\pi }$.

Asymptotically (i.e., in the limit ${\displaystyle r\rightarrow \infty }$) the metric looks like

${\displaystyle ds^{2}=dr^{2}+{\frac {r^{2}}{4}}\sigma _{3}^{2}+{\frac {r^{2}}{4}}(\sigma _{1}^{2}+\sigma _{2}^{2})}$

which naively seems as the flat metric on R4. However, for ${\displaystyle a\neq 0}$, ${\displaystyle \psi }$ has only half the usual periodicity, as we have seen. Thus the metric is asymptotically R4 with the identification ${\displaystyle \psi \,{\sim }\,\psi +2\pi }$, which is a Z2 subgroup of SO(4), the rotation group of R4. Therefore, the metric is said to be asymptotically R4/Z2.

There is a transformation to another coordinate system, in which the metric looks like

${\displaystyle ds^{2}={\frac {1}{V(\mathbf {x} )}}(d\psi +{\boldsymbol {\omega }}\cdot d\mathbf {x} )^{2}+V(\mathbf {x} )d\mathbf {x} \cdot d\mathbf {x} ,}$

where ${\displaystyle \nabla V=\pm \nabla \times {\boldsymbol {\omega }},\quad V=\sum _{i=1}^{2}{\frac {1}{|\mathbf {x} -\mathbf {x} _{i}|}}.}$

(For a = 0, ${\displaystyle V={\frac {1}{|\mathbf {x} |}}}$, and the new coordinates are defined as follows: one first defines ${\displaystyle \rho =r^{2}/4}$ and then parametrizes ${\displaystyle \rho }$, ${\displaystyle \theta }$ and ${\displaystyle \phi }$ by the R3 coordinates ${\displaystyle \mathbf {x} }$, i.e. ${\displaystyle \mathbf {x} =(\rho \sin \theta \cos \phi ,\rho \sin \theta \sin \phi ,\rho \cos \theta )}$).

In the new coordinates, ${\displaystyle \psi }$ has the usual periodicity ${\displaystyle \psi \ {\sim }\ \psi +4\pi .}$

One may replace V by

${\displaystyle \quad V=\sum _{i=1}^{n}{\frac {1}{|\mathbf {x} -\mathbf {x} _{i}|}}.}$

For some n points ${\displaystyle \mathbf {x} _{i}}$, i = 1, 2..., n. This gives a multi-center Eguchi–Hanson gravitational instanton, which is again smooth everywhere if the angular coordinates have the usual periodicities (to avoid conical singularities). The asymptotic limit (${\displaystyle r\rightarrow \infty }$) is equivalent to taking all ${\displaystyle \mathbf {x} _{i}}$ to zero, and by changing coordinates back to r, ${\displaystyle \theta }$ and ${\displaystyle \phi }$, and redefining ${\displaystyle r\rightarrow r/{\sqrt {n}}}$, we get the asymptotic metric

${\displaystyle ds^{2}=dr^{2}+{\frac {r^{2}}{4}}\left({d\psi \over n}+\cos \theta \,d\phi \right)^{2}+{\frac {r^{2}}{4}}[(\sigma _{1}^{L})^{2}+(\sigma _{2}^{L})^{2}].}$

This is R4/Zn = C2/Zn, because it is R4 with the angular coordinate ${\displaystyle \psi }$ replaced by ${\displaystyle \psi /n}$, which has the wrong periodicity (${\displaystyle 4\pi /n}$ instead of ${\displaystyle 4\pi }$). In other words, it is R4 identified under ${\displaystyle \psi \ {\sim }\ \psi +4\pi k/n}$, or, equivalently, C2 identified under zi ~ ${\displaystyle e^{2\pi ik/n}}$ zi for i = 1, 2.

To conclude, the multi-center Eguchi–Hanson geometry is a Kähler Ricci flat geometry which is asymptotically C2/Zn. According to Yau's theorem this is the only geometry satisfying these properties. Therefore, this is also the geometry of a C2/Zn orbifold in string theory after its conical singularity has been smoothed away by its "blow up" (i.e., deformation).[1]

### Gibbons–Hawking multi-centre metrics

${\displaystyle ds^{2}={\frac {1}{V(\mathbf {x} )}}(d\tau +{\boldsymbol {\omega }}\cdot d\mathbf {x} )^{2}+V(\mathbf {x} )d\mathbf {x} \cdot d\mathbf {x} ,}$

where

${\displaystyle \nabla V=\pm \nabla \times {\boldsymbol {\omega }},\quad V=\varepsilon +2M\sum _{i=1}^{k}{\frac {1}{|\mathbf {x} -\mathbf {x} _{i}|}}.}$

${\displaystyle \epsilon =1}$ corresponds to multi-Taub–NUT, ${\displaystyle \epsilon =0}$ and ${\displaystyle k=1}$ is flat space, and ${\displaystyle \epsilon =0}$ and ${\displaystyle k=2}$ is the Eguchi–Hanson solution (in different coordinates).

## References

1. ^ Douglas, Michael R.; Moore, Gregory (1996). "D-branes, Quivers, and ALE Instantons". arXiv:.