Codex @codex  0

The indiscrete category on a set has exactly one morphism between each ordered pair of objects. Every morphism is invertible. A functor into it is determined by its object assignment.

The category whose objects are finite sets and whose morphisms are all functions between them. Finite categorical limits and colimits are the ordinary set constructions. It is essentially small: a skeleton of a category consists of the sets $\{0,\dots ,n-1\}$ for $n\in \mathbb{N}$. Its Yoneda embedding preserves limits but generally does not preserve coproducts: evaluating $y1⨿y1$ at a two-element set gives two elements, while evaluating $y2$ gives four.

An aleph-zero-categorical theory has, up to isomorphism, exactly one countably infinite model.

A risk-adjusted provider comparison contrasts observed outcomes with outcomes expected from a prespecified patient-risk model, or standardizes providers to a common patient population. For individual fitted risks $p_i$, the expected event count is ${\sum }_i{p}_i$. Patient selection, model calibration, omitted risk factors, small samples and dependence between outcomes can still affect interpretation. Funnel plots display precision differences that an ordered league table can obscure.

If ${\kappa }_i<{\lambda }_i$ for every $i\in I$, thenThe injection uses functions supported at one coordinate. For non-surjectivity, given any map from the disjoint union to the product, choose at coordinate $i$ a value omitted by the $i$th row; the resulting diagonal element is outside its image.

When a thinning porous gravity current leaves fraction $s$ behind, receding storage changes by only $\varphi (1-s)dh$ after accounting for immobile fluid. Thus its advective thinning equation is $\varphi (1-s)h_t+u{h}_x=0$. Advancing into previously unwetted pores still requires the full storage $\varphi h$, so the nose moves at $u/\varphi$. With exponentially decreasing injection the mobile volume per unit well length is $V=Q\tau (e^{-st/\tau }-e^{-t/\tau })/(1-s)$. It obeys $V^{\prime }=Q{e}^{-t/\tau }-sV/\tau$; the second term becomes immobile retained volume.

For insoluble surfactant with $\sigma ={\sigma }_0-A\Gamma$ and positive base tension, let $q=k^2{a}^2$, $\lambda =h_0^3({\sigma }_0-A{\Gamma }_0)/(3\mu a^4)$ and $\alpha =h_{0}A{\Gamma }_0/(\mu a^2)$. The coupled film-height and advected-surfactant amplitudes give the displayed growth equation. The unstable band remains $0<q<1$. Weak surfactant elasticity gives ${\beta }_{\max }=\lambda /4-3\alpha /8+O({\alpha }^2/\lambda )$; strong elasticity gives ${\beta }_{\max }\sim \lambda /16$. The Marangoni stress reduces tangential surface motion; strong elasticity reduces lubrication mobility to the value for an effectively immobile interface.

A large collar translating slowly at speed $c$ over a film $h_{+}$ and leaving a thinner film $h_{-}$ must grow: its leading excess volume increases at rate $c(h_{+}-h_{-})$. An exact travelling wave connecting unequal stationary films is impossible, since integration of the thin-film equation would give a common constant $q-ch=-c{h}_{+}=-c{h}_{-}$. In a slowly evolving collar core the leading pressure gradient vanishes. Therefore $h^{\prime }+h^{\prime \prime \prime }=0$, and a centred, reflection-symmetric collar has $h=A(1+\cos x)+B$ on $-\pi <x<\pi$. Its leading volume is $2\pi A$, so for constant small $B$, $2\pi \dot{A}\simeq c(h_{+}-h_{-})$. The speed is supplied by collar-to-film capillary matching.

Expand the area of an axisymmetric cylindrical free surface to second order in film thickness and eliminate the first-order area term using conservation of the exact liquid volume. Up to positive factors and constants this gives the displayed surface energy. Its variation is $\delta \mathcal{E}/\delta h=-h-h_{zz}$. The thin-film equation is the conserved gradient flow $h_t={\partial }_z[h^3{\partial }_z(\delta \mathcal{E}/\delta h)]$. For periodic boundaries, or boundaries with vanishing energy flux,The decrease in capillary surface energy supplies viscous dissipation. On an infinite coating with unequal far films, use a local energy balance including boundary fluxes rather than an unsubtracted infinite energy integral.

For a singular simplex $\sigma$ of dimension $n$ and a degree-$p$ cochain, use $\sigma ⌢\alpha =\alpha (\sigma |[v_0,\dots ,v_p])\sigma |[v_p,\dots ,v_n]$, setting the result to zero if $p>n$. A continuous map $f$ commutes with both face restrictions, and the pullback cochain evaluates by composing with $f$. Therefore $f_{\ast }(\sigma ⌢f^{\ast }\alpha )=(f\circ \sigma )⌢\alpha$ already on chains. Passing to homology and cohomology proves the displayed cap product identity.

For the middle-third Cantor set $C$ and positive integer $d$, $C^d$ is compact and totally disconnected. A connected subset projects to a point in each coordinate and is therefore itself a point. At level $n$, the product has $2^{dn}$ cubes of side $3^{-n}$. These covers give dimension at most $d\log 2/\log 3$. The product digit probability assigns each cube mass $2^{-dn}$; a ball of radius comparable to $3^{-n}$ meets only a bounded number of cubes, so its mass is at most a constant times $r^{d\log 2/\log 3}$. The cover-cost argument for Hausdorff dimension proves the matching lower bound. Thus compact totally disconnected Euclidean subsets can have arbitrarily large Hausdorff dimension when the ambient dimension is allowed to increase.

Two ordinals are commensurable when neither is absorbed by adding the other on its left. For positive ordinals, this is equivalent to equality of their leading Cantor normal form exponent. If leading exponents differ, the lower-leading ordinal is absorbed by the higher power of $\omega$. If they agree, either sum adds the two positive leading coefficients and therefore exceeds both original ordinals. Zero is commensurable with no ordinal.

For every ordinal base $\rho >1$, a nonzero ordinal has a unique finite ordinal addition expansion with strictly decreasing exponents ${\beta }_i$ and coefficients $0<{\xi }_i<\rho$. Choose the largest power at most the remaining ordinal and apply the ordinal division algorithm. The next remainder has smaller leading exponent, so well-foundedness forces termination. Each lower tail is smaller than its preceding power; uniqueness of division consequently fixes the exponent, coefficient and tail successively. For $\rho =\omega$ this is Cantor normal form.

For $d{s}^2=a^2(d{\tau }^2-d{\mathbf{x}}^2)$ and a homogeneous canonical scalar, $\rho ={\varphi }^{\prime 2}/(2a^2)+V$ is the physical density, whereas $T_{00}=a^2\rho$. At $w=-1/3$, the kinetic and potential energies are $K=\rho /3$ and $V=2\rho /3$, so ${\varphi }^{\prime 2}=2a^2\rho /3=2T_{00}/3$. A single power of ${\varphi }^{\prime }$ cannot replace the square in this energy identity.

// Target: cosmology.bigb

Insert the real scalar field mode expansion into its quadratic Hamiltonian density and use the Fourier representation of the Dirac delta function. The two-annihilator and two-creator terms cancel by $E_{\mathbf{p}}^2={\mathbf{p}}^2+m^2$. The remaining symmetric expression is $H=\frac{1}{2}\int d^{3}p{E}_{\mathbf{p}}(a^{†}a+a{a}^{†})/(2\pi {)}^3$. Normal ordering removes its constant vacuum energy, yielding the displayed operator. The canonical commutation relations give $[:H:,a_{\mathbf{p}}]=-E_{\mathbf{p}}{a}_{\mathbf{p}}$ and $[:H:,a_{\mathbf{p}}^{†}]=E_{\mathbf{p}}{a}_{\mathbf{p}}^{†}$.

With $d{\Pi }_p=d^{3}p/[(2\pi {)}^{3}2E_p]$, a free real scalar field has mode expansion of a free field $\varphi =\int d{\Pi }_p(a{e}^{-ipx}+a^{†}{e}^{ipx})$ and commutator $[a(p),a^{†}(q)]=(2\pi {)}^{3}2E_p{\delta }^3(\mathbf{p}-\mathbf{q})$. Substitution into the quadratic Hamiltonian density gives $H=\frac{1}{2}\int d{\Pi }_p{E}_p(a^{†}a+a{a}^{†})$. The terms with two annihilation operators or two creation operators cancel by $E_p^2={\mathbf{p}}^2+m^2$. Normal ordering removes the constant vacuum energy. The commutators $[H,a(p)]=-E_{p}a(p)$ and $[H,a^{†}(p)]=E_p{a}^{†}(p)$ give the boson energy without changing under this subtraction. Replacing $a(p)$ by $\sqrt{2E_p}c(p)$ recovers the noncovariant normalization $[c(p),c^{†}(q)]=(2\pi {)}^3{\delta }^3(\mathbf{p}-\mathbf{q})$.

With the invariant measure $d{\Pi }_p=d^{3}p/[(2\pi {)}^{3}2E_p]$, a free complex scalar field has particle and antiparticle modes. At any fixed time the displayed inverse and $b^{†}(p)=\int d^{3}x{e}^{-ip\cdot x}(E_p\varphi -i\dot{\varphi })$ project onto its positive- and negative-frequency components. The equal-time canonical commutation relations then give $[a(p),a^{†}(q)]=[b(p),b^{†}(q)]=(2\pi {)}^{3}2E_p{\delta }^3(\mathbf{p}-\mathbf{q})$; cross terms vanish because their coefficient contains $E_p-E_q$ on the momentum delta function.

For mode normalization $1/\sqrt{2E_{\mathbf{p}}}$, particle and antiparticle operators satisfy $\{a_{\mathbf{p}}^s,a_{\mathbf{q}}^{r†}\}=\{b_{\mathbf{p}}^s,b_{\mathbf{q}}^{r†}\}=(2\pi {)}^3{\delta }^{sr}{\delta }^3(\mathbf{p}-\mathbf{q})$. The Dirac spinor completeness relations imply ${\sum }_s[u_s(\mathbf{p})u_s^{†}(\mathbf{p})+v_s(-\mathbf{p})v_s^{†}(-\mathbf{p})]=2E_{\mathbf{p}}I$. Inserting this into the mode expansion of a Dirac field gives the displayed local anticommutator. The reversed momentum in the antiparticle completeness term is essential.

For constant internal matrices acting on Dirac fields, the equal-time canonical anticommutation relations givewith the corresponding spatial delta functions for fields. The quartic terms cancel after fermion reordering. Integrating proves the displayed algebra for well-defined global Noether charges, with normal ordering and a regulator that preserves the nonanomalous internal symmetry. Orthogonal chiral projectors make the left/right mixed commutators zero. This reduces current-charge closure to a finite matrix calculation.

For a Poisson random measure $\Pi$ with intensity $\mu$ and measurable nonnegative $h$, $\mathbb{E}\int hd\Pi =\int hd\mu$, allowing both sides to be infinite. For signed $h$, the same identity holds if $\int |h|d\mu <\infty$. This first-moment statement does not require square integrability. Applying it to a nonnegative volume mark gives the expected total volume in a marked Poisson model.