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A Riemannian or pseudo-Riemannian metric is Einstein when its Ricci tensor is a constant scalar multiple of the metric. Constant-sectional-curvature metrics satisfy this condition with $\Lambda =(d-1)k$. The Killing-form metric on a real semisimple Lie group is another example, with $\Lambda =-1/4$ for $g=B$ in the curvature convention $R(X,Y)Z={\nabla }_X{\nabla }_{Y}Z-{\nabla }_Y{\nabla }_{X}Z-{\nabla }_{[X,Y]}Z$.

An affine connection on the tangent bundle of a smooth manifold assigns a vector field ${\nabla }_{X}Y$ to two vector fields, is $\mathbb{R}$-bilinear, and satisfiesThus its first slot is tensorial and its second obeys the Leibniz rule. Its action on covectors is defined by differentiating the pairing, and this extends it to tensor fields. A torsion-free connection has ${\nabla }_{X}Y-{\nabla }_{Y}X=[X,Y]$.

Assume that $g$ is a smooth nondegenerate metric tensor. Metric compatibility and a vanishing torsion tensor imply the Koszul formula,The right-hand side is determined by $g$ and the Lie bracket of vector fields. Nondegeneracy determines ${\nabla }_{X}Y$ uniquely; conversely this formula defines an affine connection with both required properties, proving existence as well as uniqueness. In a coordinate frame the brackets vanish. Combining the three differentiated metric tensor identities givesThis is the Levi-Civita connection. Positive definiteness is unnecessary: the argument also works for a pseudo-Riemannian metric.

For the other affine connection define $S(X,Y)={\bar{\nabla }}_{X}Y-{\nabla }_{X}Y$. The derivative of $f$ cancels between the two Leibniz rules, so $S$ is $C^{\infty }$-linear in both slots. The difference of affine connections is a tensor: here $S$ is a section of $TM\otimes T^{\ast }M\otimes T^{\ast }M$ with components ${\bar{\Gamma }}^a{}_{bc}-{\Gamma }^a{}_{bc}$. Both affine connections are torsion-free, so $S(X,Y)=S(Y,X)$.

Agreement of geodesics means agreement of their unparametrized curves; different affine parameters are allowed. For every nonzero tangent vector $v$, existence of a geodesic with that initial velocity implies that $S(v,v)$ is parallel to $v$. The symmetric bilinear diagonal-parallel lemma now determines $S$. Choose a basis $e_i$ and write $S(e_i,e_i)={\alpha }_i{e}_i$. Applying the parallelism condition to $e_i+e_j$ and $e_i-e_j$ givesWith $V(e_i)={\alpha }_i/2$, bilinearity yieldsThis is projective equivalence of affine connections. It also covers dimension one. For two Levi-Civita connections, the projective covector from metric volume densities gives the explicit answerIndeed ${\Gamma }^a{}_{ac}={\partial }_c\log \sqrt{|\det g|}$. The determinant ratio is a scalar, so this expression is a genuine covector, although either determinant alone is coordinate-dependent. This determinant expression requires nondegeneracy of $\bar{g}$; the difference-tensor and earlier trace formula require only the two torsion-free affine connections.

Conversely, the displayed tensor gives ${\bar{\nabla }}_{\dot{\gamma }}\dot{\gamma }=2V(\dot{\gamma })\dot{\gamma }$ along an affinely parametrized $\nabla$-geodesic. Choosing a new parameter $t(\tau )$ satisfying $t^{\prime \prime }/t^{\prime }=2V(\dot{\gamma })$ removes that tangential acceleration. This geodesic reparametrization under projective equivalence proves sufficiency. If agreement were required with the very same affine parameter, polarization would instead force $S=0$ and $V=0$.

For the Lie algebra $\mathfrak{g}$ of a Lie group $G$, let ${\mathrm{ad}}_X(Y)=[X,Y]$. The Killing form is the symmetric bilinear formFor a finite-dimensional real Lie algebra, the Cartan criterion for semisimplicity says that $B$ is nondegenerate precisely when $\mathfrak{g}$ is a semisimple Lie algebra. Thus a semisimple Lie group supplies the required condition. Compactness alone is insufficient: an abelian Lie algebra, including that of a torus, has zero Killing form.

The Jacobi identity gives ${\mathrm{ad}}_{[Z,X]}=[{\mathrm{ad}}_Z,{\mathrm{ad}}_X]$. Cyclic invariance of the trace therefore givesThere is also invariance under the full Adjoint representation of a Lie group: ${\mathrm{ad}}_{{\mathrm{Ad}}_{a}X}={\mathrm{Ad}}_a{\mathrm{ad}}_X{\mathrm{Ad}}_{a^{-1}}$, so $B({\mathrm{Ad}}_{a}X,{\mathrm{Ad}}_{a}Y)=B(X,Y)$.

Define a pseudo-Riemannian metric by translating $B$ from the identity:It is smooth and nondegenerate. Left translations preserve it by construction. Right translation, expressed in left-translated tangent coordinates, acts by ${\mathrm{Ad}}_{b^{-1}}$, so it also preserves the metric. This constructs a bi-invariant pseudo-Riemannian metric.

For left-invariant vector fields, the derivative terms in the Koszul formula vanish. Invariance of $B$ then givesUse the Riemann curvature tensor convention $R(X,Y)Z={\nabla }_X{\nabla }_{Y}Z-{\nabla }_Y{\nabla }_{X}Z-{\nabla }_{[X,Y]}Z$. Substituting the Levi-Civita connection and using the Jacobi identity yieldsThe Ricci tensor is the trace of $X\mapsto R(X,Y)Z$. Since $[[X,Y],Z]={\mathrm{ad}}_Z{\mathrm{ad}}_{Y}X$, it follows thatThis is the Killing-form Einstein metric. Rescaling to $g=cB$, with nonzero constant $c$, gives Einstein metric constant $-1/(4c)$.

For a compact semisimple Lie group, $B$ is negative definite and $-B$ is a positive-definite bi-invariant Riemannian metric. For example, $SU(2)$ has topology $S^3$ and metric signature $(0,3)$ for $B$, while $SO(3)$ has the same Lie algebra and metric signature, but topology ${\mathbb{RP}}^3$. The special linear group $SL(2,\mathbb{R})$ has metric signature $(2,1)$ and topology $S^1\times {\mathbb{R}}^2$; its universal covering Lie group has topology ${\mathbb{R}}^3$ and the same Killing form. The real Lie algebra of $SL(2,\mathbb{C})$ has metric signature $(3,3)$, and the group has topology $S^3\times {\mathbb{R}}^3$. Thus the Killing form distinguishes compact from noncompact directions in these semisimple examples, but does not determine global topology or distinguish different covering groups.

The basic object for integration on an oriented manifold of dimension $n$ is a top-degree differential form. In an orientation-preserving chart, write $\alpha =f(x)d{x}^1\wedge \cdots \wedge d{x}^n$. Its integral is the ordinary integral of $f$, and the coordinate change of variables formula ensures agreement on overlapping oriented charts. A partition of unity combines these local integrals into a global one, provided the form has compact support or satisfies appropriate convergence conditions. Reversing orientation reverses the integral. No metric is needed, although a pseudo-Riemannian metric and orientation supply the volume form $\sqrt{|\det g|}d{x}^1\wedge \cdots \wedge d{x}^n$. On a nonorientable manifold one instead integrates densities, or appropriately twisted top forms.

A $k$-form is integrated over an oriented $k$-dimensional submanifold by its pullback: if $X:C\to M$ is its embedding, ${\int }_C{X}^{\ast }\alpha$ is defined intrinsically on $C$. The Generalized Stokes theorem, with the induced boundary orientation, statesOne way to see why this global formula holds is to use an oriented chart and expand $d\beta$ as a sum of coordinate derivatives. The ordinary fundamental theorem of calculus gives the boundary contributions with their orientation signs. A partition of unity reduces the manifold to such charts; the artificial internal boundary contributions cancel, leaving only the actual boundary. Compactness or compact support controls the sums and the boundary at infinity.

This immediately explains how closed differential forms yield conservation laws. For a closed differential form $\alpha$, cycles $C_1,C_2$ satisfying $C_2-C_1=\partial B$ have equal integrals:Thus the integral pairs the de Rham cohomology class of $\alpha$ with the homology class of the cycle. An exact differential form integrates to zero on every closed cycle. A closed form need not be exact, and nonzero periods measure the global obstruction. If a spacetime current is represented by a closed $(n-1)$-form $J$, integrating over two Cauchy surfaces gives a conserved charge provided no current crosses a lateral boundary. A nonzero boundary flux must be retained in the Stokes calculation rather than silently discarded.

For a genuinely topological current, closure can follow identically from the field geometry, without the equations of motion. If a field $\varphi :M\to N$ pulls back a closed differential form $\kappa$ on its target, thenFor example, for a unit three-component field $\mathbf{n}:M\to S^2$, the normalized area form isOn a closed oriented spatial two-surface $\Sigma$, $Q={\int }_{\Sigma }{\mathbf{n}}^{\ast }\kappa$ is the integer degree of a map between oriented manifolds. Smooth evolution is a homotopy and conserves this topological charge. Singularities or flux through a spatial boundary can permit the charge to change. This is the pullback-volume representation of a topological current.

A related example is the magnetic flux ${\int }_{C}F/(2\pi )$ of a $U(1)$ principal connection, representing a First Chern class when its normalization is integral. Nonzero flux on a closed cycle requires nontrivial global bundle data or singular sources: if a single smooth global potential exists with $F=dA$, the flux on every closed cycle vanishes. This distinction is important when local differential equations are used to infer global conservation or quantization.

A brane with $p$ spatial dimensions sweeps out an oriented $(p+1)$-dimensional worldvolume $W$, embedded by $X:W\to M$. Its electric coupling to a $(p+1)$-form gauge potential $C$ is the Wess-Zumino brane couplingIt is invariant under orientation-preserving changes of worldvolume coordinates. Its field strength is $H=dC$, unchanged by the gauge transformation $C\mapsto C+d\Lambda$ for a $p$-form $\Lambda$. Since the pullback of a differential form commutes with the exterior derivative, its gauge variation isTherefore a closed brane has a gauge-invariant coupling under these transformations. For a noncompact worldvolume, support or decay conditions must also eliminate contributions at infinity.

For an open brane, the variation does not vanish automatically. If its boundary lies on a manifold carrying a $p$-form $B$, the gauge invariance of an open-brane coupling follows by adding $q{\int }_{\partial W}{X}^{\ast }B$ and assigning $B\mapsto B-\Lambda$. The two boundary variations cancel exactly with the induced orientation. Alternatively one may restrict the gauge parameter to have vanishing pullback at the boundary, if that is the chosen physical boundary condition. A particle has $p=0$ and couples by $q\int A$; a string has $p=1$ and couples to a two-form; a membrane has $p=2$ and couples to a three-form.

Finally, a gauge potential need not be globally a single differential form. Patchwise potentials and their overlap data define its global holonomy. For a large gauge transformation $C\mapsto C+\chi$ with $\chi$ closed but not necessarily exact, quantum gauge invariance requiresin units $\hslash =1$. This connects the coupling to integral periods and charge quantization. The local Stokes argument and these global period conditions are complementary: closure controls continuous conservation, while global topology controls which charges and gauge transformations are allowed.

A pseudo-Riemannian metric is a smooth nondegenerate symmetric bilinear form on every tangent space, with locally constant signature. Its positive-definite special case is a Riemannian metric. Unlike a positive-definite metric, an indefinite metric admits nonzero null vectors. In either signature its Levi-Civita connection is uniquely determined by torsion-freeness and metric compatibility.