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Under the $p$-biased product measure ${\mu }_p$ on $\{-1,1{\}}^n$, the coordinates are independent random variables with $\mathbb{P}(x_i=-1)=p$ and $\mathbb{P}(x_i=1)=1-p$. Writing $\mu =1-2p$, $\sigma =2\sqrt{p(1-p)}$, and ${\varphi }_i=(x_i-\mu )/\sigma$, the products ${\varphi }_S={\prod }_{i\in S}{\varphi }_i$ form the $p$-biased Fourier basis.

For $S\subseteq [n]$, the Walsh character on the Boolean hypercube is ${\chi }_S(x)={\prod }_{i\in S}{x}_i$, equivalently $(-1{)}^{{\sum }_{i\in S}{x}_i}$ in the zero-one convention.

Thermal conductivity is the material response coefficient in Fourier's law. For an isotropic material it is a scalar $k$, with units $\mathrm{W}{\mathrm{m}}^{-1}{\mathrm{K}}^{-1}$; larger positive $k$ means a larger conductive heat flux for the same temperature gradient. It can depend on temperature and composition. Direction-dependent response in an anisotropic material is described by a thermal conductivity tensor. The two worked examples use stipulated positive constants, rather than measured values for named materials.

Thermal conductivity describes material response, whereas thermal resistance also includes geometry: for the steady bar, $R_{\mathrm{th}}=L/(kA)$. Doubling $k$ at fixed length, cross-sectional area and end temperatures halves thermal resistance and doubles the rate of heat transfer. Doubling length changes thermal resistance without changing the material's thermal conductivity. This distinction lets a designer improve cooling either by choosing a higher thermal conductivity or by shortening and widening the path. It also explains why the less conductive layer in thermal resistance takes the greater temperature drop.

Thermal diffusivity answers a different question: how rapidly a temperature disturbance spreads. Its usual model $\kappa =k/(\rho c_p)$ also involves mass density $\rho$ and specific heat capacity $c_p$, so equal thermal conductivities need not imply equal rates of warming.

For the irreducible representation $V_n={\mathrm{Sym}}^n({\mathbb{C}}^2)$ of SU(2), the exterior square decomposes asFor $n=0$, the sum is empty and the exterior square is zero.

The Clebsch-Gordan decomposition for SU2 first gives $V_n\otimes V_n\cong {⨁}_{j=0}^n{V}_{2n-2j}$. By flip parity in the SU2 tensor square, exchanging the two tensor factors acts on the $j$th summand by $(-1{)}^j$. The exterior square is the minus-one eigenspace of this exchange, so it selects exactly the odd indices $j=2k+1$. Substitution gives the displayed formula.

For example, ${\bigwedge }^2{V}_2\cong V_2$ has dimension three, while ${\bigwedge }^2{V}_3\cong V_4\oplus V_0$ has dimension $5+1=6$, as required for the exterior square of a four-dimensional vector space.

Every nonidentity finite-order Möbius transformation has exactly two fixed points on the Riemann sphere. A transformation with one repeated fixed point is conjugate to a nontrivial translation and therefore has infinite order.

For $f(z)=(az+b)/(z+1)$, the finite fixed points are the roots ofThus a repeated fixed point or two prescribed fixed points determine $a$ and $b$ by the usual sum and product of roots.

The split stephas amplification matrixOn a common directional eigenvector its eigenvalue is $(1+\mu {\lambda }_p)/(1-\mu {\lambda }_q)$.

For $Y=n^{-1}\mathrm{Bin}(n,p)$, the score and information areConsequently one Fisher-scoring step sends every interior starting value directly to the MLE $\hat{p}=Y$.

If a continuous function $f$ satisfiesfor every smooth compactly supported test function $\eta$, then $f=0$ on $(a,b)$.

An integral matrix satisfying $A^2+A+I=0$ makes ${\mathbb{Z}}^n$ a module over the Eisenstein integers by letting the primitive cube root act as $A$. This module is finitely generated and torsion-free, hence free. Since the Eisenstein integers have integer rank two, such matrices exist only for $n=2m$; for that dimension every one is integrally conjugate to

An orthonormal eigenbasis of a linear operator is an orthonormal basis consisting of eigenvectors. Each vector can be reconstructed from its scalar components along those mutually perpendicular unit directions. With the convention that the inner product is linear in its first argument,The finite-dimensional spectral theorem supplies such a basis for a self-adjoint operator. In its two-dimensional example, the coordinates of $x=(1,0{)}^T$ are $1/\sqrt{2}$ along $e_{+}$ and $-1/\sqrt{2}$ along $e_{-}$. The operator multiplies those coordinates by $3$ and $1$, and reconstruction gives $Ax=(2,1{)}^T$.

Repeated eigenvalues permit different orthonormal choices within one eigenspace, so the basis need not be unique. The spectral projection of a self-adjoint matrix onto that entire eigenspace is unique: it keeps the geometrically meaningful component without choosing individual axes inside it.

The $E_7$ Coxeter graph is the simply-laced seven-vertex tree whose three arms have lengths $1$, $2$, and $3$. Its Coxeter Gram matrix is positive definite and has determinant $2$.

The character group $\hat{G}$ consists of the group homomorphisms $\gamma :G\to {\mathbb{C}}^{\times }$. Pointwise multiplication makes it a finite abelian group isomorphic to $G$.

In the Category of sets, filtered colimits commute with finite limits. Elements in a finite limiting diagram involve only finitely many representatives and finitely many equalities, all of which can be realized at one common stage of a filtered diagram.

A category is weakly filtered when every finite connected diagram in it admits a cocone. Equivalently, each of its connected components is a filtered category.

For a morphism of schemes $f:X\to Y$ and a point $y\in Y$, the scheme-theoretic fiber is the fiber product $X{\times }_Y\mathrm{Spec}\kappa (y)$. It remembers multiplicities and nilpotents that the underlying set-theoretic inverse image cannot detect.

Its underlying fiber is enriched with local-ring and multiplicity information.

The Fermi sea is the zero-temperature many-fermion quantum state with every one-particle state below the Fermi energy occupied and every state above it empty. For a uniform isotropic Fermi gas, the occupied region in momentum space is a solid sphere; its boundary is the Fermi surface. These are momenta, not positions: filling the sphere does not put the particles in a ball in ordinary space. Opposite momentum contributions cancel, so the gas at rest has zero total momentum even though its total kinetic energy is positive.

The filled states are forced upward in energy by the Pauli exclusion principle. This is different from the zero-point energy of one particle confined by a boundary. At fixed number density, the Fermi energy remains positive as the box grows to the thermodynamic limit, while the lowest box confinement energy tends to zero. Low-energy excitations move particles from occupied states near the Fermi surface into nearby empty states; deep states have no nearby available destination. This explains why only a small fraction of electrons contribute to the low-temperature electron heat capacity.^[ref]

For activator diffusion $D$, local linear decay $r$, and coupling $\rho (u-v)$, eliminating the fast inhibitor givesIts pattern-forming threshold is

Choose an orthonormal basis of $T_{p}M$ and put $e(\theta )=(\cos \theta ,\sin \theta )$. Away from the centre and cut locus,defines geodesic polar coordinates centred at $p$.

A normal neighbourhood of $p$ is the diffeomorphic image under ${\exp }_p$ of a star-shaped neighbourhood of $0$ in $T_{p}M$. In a sufficiently small normal ball, radial geodesics from $p$ uniquely minimize length.