Every self-map has $f^{\ast }a=\lambda a$ in the mod-two cohomology ring, with $\lambda \in {\mathbb{F}}_2$. Its mod-two Lefschetz number is $1+\lambda +\cdots +{\lambda }^{2r}$, equal to one for either value of $\lambda$. This is the reduction of the integral cellular Lefschetz number, so the latter is nonzero and a fixed point exists.

Double a compact orientable genus-zero topological surface with $g+1$ boundary circles. The resulting closed surface has genus $g$. The involution exchanging the halves fixes the seam circles and has local collar form $(s,t)\mapsto (s,-t)$. Compose it with a flow rotating each seam coordinate by a small nonzero amount, with speed supported in its collar. Equality with the initial point would force $t=0$, where the rotation is nonzero; off the collars the original reflection already has no fixed points. The new map is fixed-point-free and homotopic to the reflection through the flow. This gives a surface example in every genus where having fixed points is not a homotopy invariant.

A closed smooth manifold X embeds in Euclidean space. The double M of a closed tubular neighbourhood is a closed oriented manifold retracting onto X. If i is its inclusion and r its retraction, the fixed points of F correspond to those of f, and cyclicity of finite-dimensional trace gives $L(F)=L(f)$ from $i^{\ast }{r}^{\ast }=1$. Thus the oriented diagonal-class proof of the Lefschetz fixed-point theorem implies the theorem for possibly nonorientable X, without incorrectly treating its diagonal as cooriented.

For a real $n$-dimensional vector space of continuous functions on a compact interval, choose sites maximizing the absolute evaluation determinant in any basis. Linear independence ensures some nonzero evaluation determinant, so a maximizer exists and has distinct sites. Replacing row $i$ by evaluation at $t$ multiplies the determinant by the cardinal function ${\ell }_i(t)$. Maximality implies $|{\ell }_i(t)|\le 1$, hence the Lebesgue constant of interpolation is at most $n$. This gives a useful interpolation set without asserting that determinant maximization minimizes the Lebesgue constant of interpolation.

For metric $2(dwd\bar{w}+dzd\bar{z})$, the commutator is $[L,M]=F_{wz}+\lambda (F_{w\bar{w}}+F_{z\bar{z}})+{\lambda }^2{F}_{\bar{w}\bar{z}}$. Vanishing for every spectral parameter $\lambda$ is exactly the Anti-self-dual Yang-Mills equations. The derivative parts span a totally null two-plane in the complexified tangent space. Thus an invertible fundamental solution of $L\Psi =M\Psi =0$ exists locally exactly when the three gauge curvature coefficients vanish; compatibility of one possibly zero vector alone is not enough.

// Destination: fiber-bundle.bigb

On the zero-boundary Sobolev space $H_0^1(0,1)$ with norm $\Vert u^{\prime }{\Vert }_{L^2}$, assume measurable coefficients $0<p_0\le p\le p_1$ and $0\le q\le q_1$. The Poincaré inequality and Cauchy-Schwarz inequality give $|a(u,v)|\le (p_1+q_1/{\pi }^2)\Vert u^{\prime }{\Vert }_2\Vert v^{\prime }{\Vert }_2$, while nonnegativity of $q$ gives $a(u,u)\ge p_0\Vert u^{\prime }{\Vert }_2^2$. Thus the form is a bounded bilinear form and a coercive bilinear form. For a source in $H^{-1}$, the Lax-Milgram theorem yields a unique weak solution and every conforming Galerkin method approximation. No derivative of the bounded coefficient $p$ is needed for this weak formulation.

If two thermodynamic systems are each in thermal equilibrium with the same third system in the same equilibrium state, they are in thermal equilibrium with each other. Write $A\sim B$ for this relation. The zeroth law of thermodynamics supplies transitivity:Its symmetric relation property and self-equilibrium (reflexivity), together with transitivity, make thermal equilibrium an equivalence relation. Its equivalence classes can be labelled by a common empirical temperature; choosing an absolute numerical scale requires the further structure of thermodynamic temperature.^[ref]

The comparison assumes internally equilibrated macroscopic bodies, unchanged composition and mechanical constraints, and contact permitting only heat exchange. Use rigid, impermeable diathermal walls so that neither matter transfer nor boundary work spoils the test. The same state of $C$ matters: letting $C$ warm while measuring $A$, then cool while measuring $B$, does not supply the premise. Ordinary nonrelativistic laboratory thermodynamics is assumed; the Tolman temperature law treats gravitational qualifications. Equal temperatures establish the thermal condition, without requiring mechanical equilibrium or chemical equilibrium.

This explains why a thermometer can compare unlike materials: it supplies a reusable third system. A temperature is a property of an equilibrium state, while heat is energy transferred because of a temperature difference. Two bodies at the same temperature can have different internal energies and heat capacities. A thermometer therefore does not measure a body's stored amount of heat; the finite-body disturbance and waiting-time calculations in thermometer describe how making the comparison can change the state being measured.^[ref]

The name “zeroth” reflects logical order rather than the date of the first thermometer: this premise about thermal equilibrium precedes the already numbered first law of thermodynamics, Second law of thermodynamics and third law of thermodynamics. This is the naming explanation given in University Physics Volume 2 by Samuel J. Ling and others (§1.1, “Thermal Equilibrium”).^[ref]

The corresponding Zeroth law of black-hole mechanics states constancy of surface gravity over an equilibrium horizon; Hawking radiation identifies that quantity with physical temperature up to its universal conversion factor.

On a least-angle segment $\beta (\gamma )=\beta +\gamma d$, a nonzero active regression coefficient reaches zero at the displayed first positive root. Continue only as far as the first dropout, inactive-entry event or zero-correlation endpoint. At a dropout remove the vanishing regression coefficient from the active direction and recompute. This preserves agreement between nonzero regression coefficient signs and residual-score signs, which the Karush-Kuhn-Tucker conditions for the Lasso require. A removed regression coefficient may re-enter later; the active set need not grow monotonically.

At a positive penalty level, let $E$ be the residual-score equality set, $s_j$ its signs and $N$ the nonzero regression coefficient support. With full column rank, the displayed strictly convex quadratic program selects the direction for a small decrease of the penalty. Existing nonzero regression coefficients have unrestricted tangent components; tied zero regression coefficients may move only with their residual signs. Stationarity gives $X_j^{T}Xv=s_j$ for $j\in N$ and for entering zero coordinates, and $s_j{X}_j^{T}Xv\ge 1$ for tied coordinates that remain zero. These are exactly the first-order Karush-Kuhn-Tucker conditions for the Lasso along the next segment. Normalize $Xv$ to obtain the corresponding least-angle direction. This resolves simultaneous entries or dropouts without adding a generic-position assumption.

// Target: mathematical-optimization.bigb

The Liénard radiated-power formula gives the total instantaneous emitted power of an accelerated classical point charge. Write $\mathbf{v}$ for its velocity, $\mathbf{a}=d\mathbf{v}/dt$ for its coordinate acceleration and $\gamma$ for its Lorentz factor. In SI units,For small $\mathbf{v}/c$ this reduces to the Larmor formula. The perpendicular and parallel components carry different powers of $\gamma$, which makes the constraint in a radiation comparison important.

With metric signature $(+---)$, four-velocity $u^{\mu }$ and four-acceleration $A^{\mu }=d{u}^{\mu }/d\tau$, the same SI result isThe minus sign compensates the negative squared norm of the four-acceleration. This total emitted power is invariant under changes of inertial frame; directional detected radiative flux involves additional angle and arrival-time transformations. ^[ref]

For circular motion perpendicular to a magnetic field, $\gamma m|\mathbf{a}|=|q|vB$ givesThis substitution uses the magnetic Lorentz force and keeps the same SI units throughout.

The continuous-time diffusion model on a finite undirected graph uses the Graph Laplacian in the ordinary differential equationAcross each edge, the higher value sends an amount proportional to the difference to the lower value. The two contributions cancel in the sum over vertices, giving conservation of mass:If the entries represent masses, start with nonnegative entries; signed entries can instead describe deviations from a common level. For the three-vertex path graph, the initial vector $x(0)=(1,0,-1{)}^T$ is an eigenvector with eigenvalue one, so the exact solution isMore generally, an eigenvector with eigenvalue $\lambda$ decays by $e^{-\lambda t}$. The spectral theorem for real symmetric matrices supplies an orthonormal basis of these eigenvectors, and the kernel of a graph Laplacian identifies the surviving terms. On a nonempty connected graph,The limiting value is the original arithmetic mean. On a disconnected graph, each connected component of a graph converges to its own original arithmetic mean. The same matrix therefore measures neighbour disagreement, detects disconnected regions and governs relaxation toward agreement.

The kernel of the Graph Laplacian consists exactly of vectors constant on each connected component of a graph. Indeed, $Lx=0$ implies $x^{T}Lx=0$, so the Graph Laplacian quadratic form forces equality at the endpoints of every edge; equality then propagates along graph paths. Conversely, these equalities make every entry of $Lx$ zero. Thus the dimension of the kernel, equivalently the multiplicity of the zero eigenvalue, counts the connected components of a graph.

For the disconnected graph with just two edges, $AB$ and $CD$, in order $A,B,C,D$,The two displayed vectors form a basis of the kernel. The other two eigenvectors $(1,-1,0,0{)}^T$ and $(0,0,1,-1{)}^T$ each have eigenvalue two, so the full list of eigenvalues, including multiplicities, is $0,0,2,2$. Separate connected components of a graph allow independent constant levels; a single global constant is only one of these possibilities.

Assign a real value $x_i$ to each vertex. The Graph Laplacian quadratic form measures disagreement across edges:This makes the Graph Laplacian a positive semidefinite matrix. The energy is small when neighbours have similar values, even if distant vertices have very different values; it depends on connections rather than where the graph is drawn. In the three-vertex path graph, take $x=(2,0,-1{)}^T$. Thenand the two edges contribute $(2-0{)}^2=4$ and $(0-(-1){)}^2=1$.

For a short proof, expand $x^T(D-A)x$. Each edge contributes $x_i^2+x_j^2$ through the degree matrix and $-2x_i{x}_j$ through the adjacency matrix, yielding $(x_i-x_j{)}^2$. The sum over unordered edges has no factor $1/2$; a sum over all ordered pairs does:Equivalently, let $B$ be an oriented incidence matrix, with one row per edge. Then $Bx$ records endpoint differences and $L=B^{T}B$, independently of the chosen orientations. This translates a local comparison into a global quadratic form and makes its nonnegativity visible.

The degree matrix is the diagonal matrix whose $i$th diagonal entry is the degree of a vertex $i$. For a finite simple graph, $d_i={\sum }_j{A}_{ij}$, where $A$ is its adjacency matrix. For a Weighted graph Laplacian, use the sum of incident edge weights instead of the number of incident edges.

For nonnegative $X$ with finite second moment, differentiation under the expectation gives ${\varphi }^{\prime }(\lambda )=-\mathbb{E}[X{e}^{-\lambda X}]$ for $\lambda >0$. The exponential Taylor remainder divided by ${\lambda }^2$ tends pointwise to zero and is bounded in absolute value by $X^2/2$. The dominated convergence theorem therefore proves the displayed expansion without requiring a third moment.

For $t>0$, this Laplace transform converges at zero because $dx/[x{\log }^{2}x]$ is integrable, and at infinity because of exponential damping. Its large-$t$ behavior is governed by a logarithmic zero-endpoint singularity and begins with $1/\log t$, rather than a power of $t$.

Extend a function given for nonnegative time to the real line by setting it to zero before the starting time. This turns unilateral convolution into whole-line convolution and identifies a Laplace transform slice with a Fourier transform after exponential function weighting.

The set of complex numbers $s$ for which the displayed integral is finite is the region of absolute convergence of a Laplace transform. It depends only on the real part $\sigma =\mathrm{Re}s$. Once the condition holds for one $\sigma$, it holds for every larger real part. For the exponential function $e^{-2t}$ it is exactly $\mathrm{Re}s>-2$; in general, convergence on the boundary must be checked separately. An analytic continuation outside this set need not equal a convergent defining integral.

A function has exponential order $a\in \mathbb{R}$ if some $M>0$ and $T\ge 0$ give the displayed bound. Bounded functions, including sine, have exponential order zero; $e^{-2t}$ has exponential order $-2$. The bound need not use the smallest possible $a$. Together with piecewise continuity, it guarantees a Laplace transform for $\mathrm{Re}s>a$.

If an odd amplitude multiplies an even Gaussian phase on an interval asymmetric about its interior minimum, the symmetric central integral cancels exactly. The surviving leading term can be exponentially small and comes from the nearer unmatched endpoint. For example,An interior Laplace method expansion alone yields zero to every algebraic order and does not capture this term.