isolated sectors: production and thermalisation · supervisors: john march-russel & subir...
TRANSCRIPT
Isolated sectors: production and thermalisation
Hannah TillimSupervisors: J. March-Russell & S. West
Dalitz Seminar, University of Oxford, October 2018
Dark Matter fromPrimordial Black Holes
O. Lennon, J. March-Russell, R. Petrossian-Byrne, H. Tillim,Black Hole Genesis of Dark Matter, JCAP 1804 (2018), arXiv:1712.07664
Hannah Tillim Isolated sectors: production & thermalisation October 11, 2018 1 / 12
Isolated sector DM
• The WIMP paradigm - requires couplingsbetween sectors - much of the parameter spacenow explored
• Important to explore alternatives
“Isolated”
Interactions
with SM purely
gravitational
• Production mechanisms(freeze-out, freeze-in) notapplicable to isolated sectors
• Coupling to gravity →Hawking radiation
Hannah Tillim Isolated sectors: production & thermalisation October 11, 2018 2 / 12
Hawking radiation
Hawking temperature:
TBH =M2
Pl
8πMBH
Hawking radiation rate:
d
(dNs,i
dt
)=∑`,h
(2`+ 1)
2π
Γi,s,`,h(ω)
exp(ω/T (t)) + (−1)(2s+1)dω
S. Hawking, Commun.Math.Phys. 43 (1975) 199-220D. Page, Phys. Rev. D13 (1976) 198206
Hannah Tillim Isolated sectors: production & thermalisation October 11, 2018 3 / 12
Hawking radiation
→ Ns,i 'fs,igs,i
2eT
(M0
MPl
)2{1 (T0 > mi/ds)
d2sT
20 /m
2i (T0 < mi/ds)
eT =∑i,s
gi,sei,s
Hannah Tillim Isolated sectors: production & thermalisation October 11, 2018 4 / 12
Setup
• Model:• Population of micro pBHs with near-uniform initial density n0• Any other initial energy density is SM radiation (no DM)• DM is single species, long-lived, sub-Planckian massive
particles, spin ≤ 2
• Simplifying assumptions:• All Schwarzschild• All masses = M0
• T0 > vW
Hannah Tillim Isolated sectors: production & thermalisation October 11, 2018 5 / 12
Setup
dρBH
dt+ 3HρBH = −eT
M4Pl
M2n
dρrad
dt+ 4Hρrad = +eT
M4Pl
M2n
H(t)2 = 8π(ρBH + ρrad)/3M2Pl
dM
dt= −
M4Pl
M2
∑s,i
es,igs,i ≡ −eTM4
Pl
M2
• Fast vs. slow evaporation
• Light vs. heavy DM
• Yield Yi ≡ ni/stot
Hannah Tillim Isolated sectors: production & thermalisation October 11, 2018 6 / 12
Light DM results
Y slowi ' 1
2
fs,igs,i
g14∗ e
12T
(MPl
M0
) 12
Y fasti ' 1
2
fs,igs,i
g14∗ eT
(n0
M3Pl
) 14(M0
MPl
) 54
• Y ×mDM = 0.43 eV
Hannah Tillim Isolated sectors: production & thermalisation October 11, 2018 7 / 12
Thermalisation
Ongoing work with J. March-Russell, S. West
Hannah Tillim Isolated sectors: production & thermalisation October 11, 2018 8 / 12
Thermalisation
• Emitted with non-thermal spectrum and very high energy tail
• Underpopulated compared to equilibrium density
• Require redistribution of energy (2→ 2) and particle creation(2→ 3 ...)
Kinetic f(p) = 1/(exp[−(E − µ)/T ]± 1)Thermal Ti = TChemical
∑µini =
∑µfinj
• Other studies in this direction: S. Davidson & S. Sarkar arXiv:0009.078v3; M.Garny et. al. arXiv:1810.01428, S. Heeba; F. Kahlhoefer & P. Stocker arXiv:1809.04849, ....
Hannah Tillim Isolated sectors: production & thermalisation October 11, 2018 9 / 12
Thermalisation
• Kinetic, thermal and ‘partial chemical’ → evolution to fullchemical
• Boltzmann equation governs evolution - depends on a collisionterm we can parameterise in many classes of models as:
n+ 3Hn =g
π2An
(T
M
)αT 4(Z2 − Z3)
Z = eµ/T , Z0 << 1→ Zeq = 1
Hannah Tillim Isolated sectors: production & thermalisation October 11, 2018 10 / 12
Thermalisation: interim results
Hannah Tillim Isolated sectors: production & thermalisation October 11, 2018 11 / 12
What’s next
• Robust model-independent framework for estimatingthermalisation timescales
• Concrete pheno of permanently underpopulated sectors
• Application to pBH production model to reopen light DM case
Thank you!
Hannah Tillim Isolated sectors: production & thermalisation October 11, 2018 12 / 12
1
Rudin Petrossian-Byrne
Supervisors: John March-Russel & Subir Sarkar
October 2018
Dark matter and Baryogenesis from primordial black holes
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SM + DM from PBHs continued…Constraints: Free streaming!
Baryogenesis from Hawking radiationHR as tunnelling!
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OVERVIEW
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Constraints
Reheat temperature for BBN physics
Theoretical consistency
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Constraints: Free Streaming
For successful structure formation impose< 10% of DM relativistic when the SM plasma
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T ≈ 1 keV
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Constraints: Free Streaming
For successful structure formation impose< 10% of DM relativistic when the SM plasma T ≈ 1 keV
time
Instantaneous emission
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Constraints: Free Streaming
For successful structure formation impose< 10% of DM relativistic when the SM plasma T \sim 1 keV
time
Instantaneous emission
Integrated spectrum at
‘fast’
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Constraints: Free Streaming
For successful structure formation impose< 10% of DM relativistic when the SM plasma T \sim 1 keV
time
Instantaneous emission
Integrated spectrum at
‘fast’
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Constraints: Free Streaming
time
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Constraints: Free Streaming
time
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Constraints: Free Streaming
time
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Constraints: Free Streaming
time
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Constraints: Free Streaming
time
s=2
s=0
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Constraints: Free Streaming
s = 0, 1/2 excluded
s = 3/2 marginal at best s = 2 naively survives
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So far
mass
‘Heavy’ DM
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‘Heavy’ DM
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‘Heavy’ DM
Free streaming provides no extra constraint!
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Baryogenesis from PBHs
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Baryogenesis from PBHs
BHs violate all global charges
It is sufficient to provide an energy incentive to the BH to preferentially emit + over – charge
Environment can provide a chemical potential, e.g.Cohen & Kaplan (1988)Hook (2015)
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Hawing radiation as tunnellingParikh & Wilczek (1999)
WKB
is the classical action. horizon
r
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Hawing radiation as tunnellingParikh & Wilczek (1999)
WKB
is the classical action. horizon
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Relativistic Hamilton – Jacobi equation
Gullstrand–Painlevé time
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Hawing radiation as tunnellingParikh & Wilczek (1999)
WKB
is the classical action. horizon
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Relativistic Hamilton – Jacobi equation
Gullstrand–Painlevé time
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--
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Parikh & Wilczek (1999)
WKB
is the classical action. horizon
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Relativistic Hamilton – Jacobi equation
Hawing radiation as tunnelling
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Parikh & Wilczek (1999)
WKB
is the classical action. horizon
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Relativistic Hamilton – Jacobi equation
Hawing radiation as tunnelling
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only time derivative matters!
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Asymmetry generation
Currently & in future looking at lots of interesting phenomenology!
e.g. - asymmetric dark matter scenarios
- properties of
. . . . . . much more
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Thank you!
where’s Rudin?www.jackfm.co.uk/news
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Thank you!
www.jackfm.co.uk/newsthere’s Rudin
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Precision measurements of PDFs at the LHCSHAUN BAILEY
SUPERVISOR: LUCIAN HARLAND-LANG
1
Outline▪Basics: ▪What are PDFs?
▪Why are they useful?
▪How are PDFs fitted?
▪HL-LHC
▪𝑡 ҧ𝑡 fits
▪NNLO DIS
2
Basics
3
What are PDFs?
▪QCD factorization theorem allows us to split DIS/hadron collisions into low and high energy parts
▪Low energy is universal
▪High energy is calculable
𝑓(𝑥, 𝑄2)
ො𝜎(𝑥, 𝑄2)
4
𝑙𝑙′
𝛾/𝑊/𝑍
𝑝
𝑞
Why are PDFs useful?
gt
Ht
g g
g
X
5
High energy ⇒ high 𝑥
Resonant state
Errors increase as mass increases
How do we fit PDFs?
NNPDF MMHT CT HERA …..
HessianMonte Carlo
Global fits More restricted data sets
Theory, 𝜎 𝑥, 𝑄2
Data
𝜒2Minimise
New parameter set
Applgrid / fastNLO grid
Parameter set
ෝ𝜎 𝑥, 𝑄2
𝑓 𝑥, 𝑄2
6
HL-LHC
7
HL-LHC
▪Operating between ~ 2026-2038
▪ℒ = 3 ab−1 for ATLAS and CMS, ℒ = 0.3 ab−1 for LHCb
▪Any theory prediction will require a prediction of the PDFs at HL-LHC
8
Shortened version will appear in the HL-LHC Yellow Report
Collaboration between NNPDF, MMHT and CT
arXiv: 1810.03639
HL-LHCWant to generate pseudo-data (fake data) to quantify the predicted affect of the HL-LHC on PDFs
9
Statistics
stat ~ 𝑁
𝑁~𝑎ℒ𝜕𝜎
𝜕𝑥Δ𝑥
𝑎 = 𝐵𝑟 ×𝑁𝑜𝑏𝑠
𝑁𝑝𝑟𝑒𝑑𝑖𝑐𝑡𝑒𝑑
Systematics
𝐹 = 𝑓corr × 𝑓red
sys 14 TeV ~ 𝐹 × sys 8/13 TeV
𝑓𝑐𝑜𝑟𝑟 = 0.5, 𝑓𝑟𝑒𝑑 = 0.2 − 1 (8 TeV)
HL-LHC
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High 𝑥 gluon Strange quark
High 𝑥 gluon + valence quarks Mid 𝑥 gluon + antiquarks
Flavour separation
Mid 𝑥 gluon
Hessian Profiling
Expand theory around minimum:
𝜎𝑖 → 𝜎𝑖 +
𝛼
𝛽𝑖𝛼𝜆𝛼
Δ𝜒2 =
𝑖𝑗
𝐷𝑖 − 𝜎𝑖 −
𝛼
𝛽𝑖𝛼𝜆𝛼 cov 𝑖𝑗−1 𝐷𝑗 − 𝜎𝑗 −
𝛾
𝛽𝑗𝛾𝜆𝛾 + 𝑇2
𝛼
𝜆𝛼2
DataOther data
setsError from
data
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𝜒2 = 𝜒02 + 𝑧𝑖𝑧𝑖 𝑧𝑖 = 𝑇 → Error PDF
HL-LHC
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▪ Good overall reduction▪ Mostly independent of the value of 𝐹▪ Reduction dominated by increased statistics
*Phenomenology plots available
My work has been to:▪ Generate the pseudo-data▪ Perform the profiling
HL-LHC▪Do not know full extent of correlations
▪In reality, data sets may be inconsistent and may disagree with each other
▪We have only selected a subset of processes
▪New techniques could be developed before the HL-LHC data is released
▪New processes might be considered
▪May expand formalism to LHeC
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𝑡 ҧ𝑡
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𝑡 ҧ𝑡
gt
tg
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▪ 8TeV, lepton + jet channel at ATLAS▪ First time differential distributions
used in MMHT▪ Should constrain high 𝑥 gluon PDF
High energy
𝑡 ҧ𝑡
𝜒2/𝑁
Baseline Fit
𝑝𝑇 3.88 → 3.26
𝑦𝑡 3.41 → 2.76
𝑦𝑡 ҧ𝑡 4.77 → 3.10
𝑀𝑡 ҧ𝑡 3.41 → 2.69
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Impact at high 𝑥 Reduction of errors High 𝜒2 values
𝑡 ҧ𝑡
𝜒2/𝑁
Correlated Decorrelated
𝑝𝑇 3.26 → 0.90
𝑦𝑡 2.73 → 1.24
𝑦𝑡 ҧ𝑡 3.10 → 1.99
𝑀𝑡 ҧ𝑡 2.69 → 0.69
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𝜒2 values still highStable gluon Further reduction of errors
𝑡 ҧ𝑡▪The total rapidity data is also inconsistent with correlation model
▪Try to decorrelate along 𝑦𝑡𝑡, however unsuccessful
▪We need a more flexible description of two-point correlators
▪We can use di-lepton data which has reduced QCD related errors
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DIS
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DIS and the strange quark
μ
s,d
c
s,d
νμ μ
νμ
WW
▪ Neutrino induced DIS at CCFR/NuTeV
▪ Searching for dimuon signal▪ Tension with ATLAS W/Z data▪ New NNLO calculations could
resolve this?
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DIS: GM-VFS▪Two different schemes
▪FFS – No charm PDF, production of charm only through gluon
▪ZM-VFS – Charm PDF included
▪Need to combine both but NNLO calculation only for FFS
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μνμ
W
W
μ
νμ
s,d
s,dc
c
g𝑚𝑐 ∼ 𝑄
𝑚𝑐 ≪ 𝑄
Thanks for you attention
Any questions?
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Backup slides
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Pheno - Higgs
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Pheno – Dijets + Diphoton
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Pheno – supersymmetry
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Luminosities
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2d Quantum Gravity and Matter
Praveen Xavier
October 11, 2018
Introduction
I Lorentzian GR has a causal structure
(i.e it has no closedtime-like or null paths and any causal diamond between twopoints has no ”missing points”).
I Such space-times are said to be globally hyperbolic.
I For the theory of QG to have a semi-classical limit with thisbehaviour, it might be a good idea to build this feature intothe space-times in the path integral. So, we consider onlyglobally hyperbolic spacetimes in the path integral.
Introduction
I Lorentzian GR has a causal structure (i.e it has no closedtime-like or null paths and any causal diamond between twopoints has no ”missing points”).
I Such space-times are said to be globally hyperbolic.
I For the theory of QG to have a semi-classical limit with thisbehaviour, it might be a good idea to build this feature intothe space-times in the path integral. So, we consider onlyglobally hyperbolic spacetimes in the path integral.
Introduction
I Lorentzian GR has a causal structure (i.e it has no closedtime-like or null paths and any causal diamond between twopoints has no ”missing points”).
I Such space-times are said to be globally hyperbolic.
I For the theory of QG to have a semi-classical limit with thisbehaviour, it might be a good idea to build this feature intothe space-times in the path integral. So, we consider onlyglobally hyperbolic spacetimes in the path integral.
Introduction
I Lorentzian GR has a causal structure (i.e it has no closedtime-like or null paths and any causal diamond between twopoints has no ”missing points”).
I Such space-times are said to be globally hyperbolic.
I For the theory of QG to have a semi-classical limit with thisbehaviour, it might be a good idea to build this feature intothe space-times in the path integral.
So, we consider onlyglobally hyperbolic spacetimes in the path integral.
Introduction
I Lorentzian GR has a causal structure (i.e it has no closedtime-like or null paths and any causal diamond between twopoints has no ”missing points”).
I Such space-times are said to be globally hyperbolic.
I For the theory of QG to have a semi-classical limit with thisbehaviour, it might be a good idea to build this feature intothe space-times in the path integral. So, we consider onlyglobally hyperbolic spacetimes in the path integral.
Time slices
If the space-time is globally hyperbolic, there must exist a causalcurve connecting any point to an initial-value space-likehypersurface.
Figure: A causal curve connecting the point P to a space-likehypersurface
Time slices
If the space-time is globally hyperbolic, there must exist a causalcurve connecting any point to an initial-value space-likehypersurface.
Figure: A causal curve connecting the point P to a space-likehypersurface
I Vice versa, all points can be reached by evolving aninitial-value hypersurface in time.
I It’s then clear that such a space-time will possess a global,proper-time slicing.
Figure: Proper-time slices
I Vice versa, all points can be reached by evolving aninitial-value hypersurface in time.
I It’s then clear that such a space-time will possess a global,proper-time slicing.
Figure: Proper-time slices
2d
My work has been in 2d. So let’s specialize and consider thismodel in 2d.
The action in 2d is:
S = −λVolM + topological term
To discretize, we propose to construct the surface using
I flat equilateral Lorentzian triangles
with 1 space-like edge (of length-squared a2) and 2 time-likeedges (of length squared −a2).
I This model of QG (without matter) in 2d is called the CausalDynamical Triangulation (CDT) model.
2d
My work has been in 2d. So let’s specialize and consider thismodel in 2d. The action in 2d is:
S = −λVolM + topological term
To discretize, we propose to construct the surface using
I flat equilateral Lorentzian triangles
with 1 space-like edge (of length-squared a2) and 2 time-likeedges (of length squared −a2).
I This model of QG (without matter) in 2d is called the CausalDynamical Triangulation (CDT) model.
2d
My work has been in 2d. So let’s specialize and consider thismodel in 2d. The action in 2d is:
S = −λVolM + topological term
To discretize, we propose to construct the surface using
I flat equilateral Lorentzian triangles
with 1 space-like edge (of length-squared a2) and 2 time-likeedges (of length squared −a2).
I This model of QG (without matter) in 2d is called the CausalDynamical Triangulation (CDT) model.
2d
My work has been in 2d. So let’s specialize and consider thismodel in 2d. The action in 2d is:
S = −λVolM + topological term
To discretize, we propose to construct the surface using
I flat equilateral Lorentzian triangles
with 1 space-like edge (of length-squared a2) and 2 time-likeedges (of length squared −a2).
I This model of QG (without matter) in 2d is called the CausalDynamical Triangulation (CDT) model.
2d
My work has been in 2d. So let’s specialize and consider thismodel in 2d. The action in 2d is:
S = −λVolM + topological term
To discretize, we propose to construct the surface using
I flat equilateral Lorentzian triangles
with 1 space-like edge (of length-squared a2) and 2 time-likeedges (of length squared −a2).
I This model of QG (without matter) in 2d is called the CausalDynamical Triangulation (CDT) model.
2d
We start with a discrete initial line:
2d
We start with a discrete initial line:
2d
We start with a discrete initial line: Then we add our flatequilateral triangles to evolve the line to one at a later time:
2d
We start with a discrete initial line: Then we add our flatequilateral triangles to evolve the line to one at a later time:
2d
We start with a discrete initial line: Then we add our flatequilateral triangles to evolve the line to one at a later time:
2d
We start with a discrete initial line: Then we add our flatequilateral triangles to evolve the line to one at a later time:
The area of one of these fundamental triangles is A =√
5a2
4 .
Therefore, the discrete version of the action is:
Sdscrte = −λN(T )A
where N(T ) is the number of triangles of the triangulation T .
I The geodesic distance is the shortest graph distancebetween any two points. Hence, each triangulation uniquelyspecifies an equivalence class of metric configurations.
The area of one of these fundamental triangles is A =√
5a2
4 .Therefore, the discrete version of the action is:
Sdscrte = −λN(T )A
where N(T ) is the number of triangles of the triangulation T .
I The geodesic distance is the shortest graph distancebetween any two points. Hence, each triangulation uniquelyspecifies an equivalence class of metric configurations.
The area of one of these fundamental triangles is A =√
5a2
4 .Therefore, the discrete version of the action is:
Sdscrte = −λN(T )A
where N(T ) is the number of triangles of the triangulation T .
I The geodesic distance is the shortest graph distancebetween any two points. Hence, each triangulation uniquelyspecifies an equivalence class of metric configurations.
The area of one of these fundamental triangles is A =√
5a2
4 .Therefore, the discrete version of the action is:
Sdscrte = −λN(T )A
where N(T ) is the number of triangles of the triangulation T .
I The geodesic distance is the shortest graph distancebetween any two points. Hence, each triangulation uniquelyspecifies an equivalence class of metric configurations.
Matter and DimersClassically, matter couples to the geometry via the metric and itsdescendants.
We propose to imitate matter at the classical level,by placing ”dimers” across two triangles, with the rule that theycannot meet on the face of any triangle.
I The latter rule ensures that the new degrees of freedomcouple to the geometry of the triangulation. Such dimers arereferred to as hard.
I Let’s refer to this dimer model as CDT-D
Matter and DimersClassically, matter couples to the geometry via the metric and itsdescendants. We propose to imitate matter at the classical level,by placing ”dimers” across two triangles, with the rule that theycannot meet on the face of any triangle.
I The latter rule ensures that the new degrees of freedomcouple to the geometry of the triangulation. Such dimers arereferred to as hard.
I Let’s refer to this dimer model as CDT-D
Matter and DimersClassically, matter couples to the geometry via the metric and itsdescendants. We propose to imitate matter at the classical level,by placing ”dimers” across two triangles, with the rule that theycannot meet on the face of any triangle.
I The latter rule ensures that the new degrees of freedomcouple to the geometry of the triangulation. Such dimers arereferred to as hard.
I Let’s refer to this dimer model as CDT-D
Matter and DimersClassically, matter couples to the geometry via the metric and itsdescendants. We propose to imitate matter at the classical level,by placing ”dimers” across two triangles, with the rule that theycannot meet on the face of any triangle.
I The latter rule ensures that the new degrees of freedomcouple to the geometry of the triangulation. Such dimers arereferred to as hard.
I Let’s refer to this dimer model as CDT-D
Dimer action
In the presence of dimers, we add to the action a termproportional to the number of dimers:
S = −λN(T )A+αN(D)
where N(D) is the number of dimers of a dimer configuration D.Therefore, the weight of a CDT-D configuration is:
Exp(iS) = Exp [−iλN(T )A + iαN(D)] =: gN(T )ξN(D)
where, g := Exp(−iλA) and ξ := Exp (iα)
Dimer action
In the presence of dimers, we add to the action a termproportional to the number of dimers:
S = −λN(T )A+αN(D)
where N(D) is the number of dimers of a dimer configuration D.
Therefore, the weight of a CDT-D configuration is:
Exp(iS) = Exp [−iλN(T )A + iαN(D)] =: gN(T )ξN(D)
where, g := Exp(−iλA) and ξ := Exp (iα)
Dimer action
In the presence of dimers, we add to the action a termproportional to the number of dimers:
S = −λN(T )A+αN(D)
where N(D) is the number of dimers of a dimer configuration D.Therefore, the weight of a CDT-D configuration is:
Exp(iS)
= Exp [−iλN(T )A + iαN(D)] =: gN(T )ξN(D)
where, g := Exp(−iλA) and ξ := Exp (iα)
Dimer action
In the presence of dimers, we add to the action a termproportional to the number of dimers:
S = −λN(T )A+αN(D)
where N(D) is the number of dimers of a dimer configuration D.Therefore, the weight of a CDT-D configuration is:
Exp(iS) = Exp [−iλN(T )A + iαN(D)]
=: gN(T )ξN(D)
where, g := Exp(−iλA) and ξ := Exp (iα)
Dimer action
In the presence of dimers, we add to the action a termproportional to the number of dimers:
S = −λN(T )A+αN(D)
where N(D) is the number of dimers of a dimer configuration D.Therefore, the weight of a CDT-D configuration is:
Exp(iS) = Exp [−iλN(T )A + iαN(D)] =: gN(T )ξN(D)
where, g := Exp(−iλA) and ξ := Exp (iα)
Partition Function
The partition function (PF) of this model is the sum of theweight over all possible CDT-D configurations:
Z (g , ξ) =∑{T ,D}
gN(T )ξN(D) =∑
k
gk
∑l
ξl∑{Tk ,Dl}
1
where {T ,D} is the set of all CDT-D configurations and {Tk ,Dl}
is the set of CDT-D configs. with k triangles and l dimers.
I The radius of convergence of the power sum in g is it’scritical value denoted gc(ξ).
I At gc(ξ), the PF, Z (gc , ξ) behaves non-analytically.
I A critical point can be characterized by it’s Hausdorffdimension dH:
〈Area(R)〉∝RdH
Partition Function
The partition function (PF) of this model is the sum of theweight over all possible CDT-D configurations:
Z (g , ξ) =∑{T ,D}
gN(T )ξN(D) =
∑k
gk
∑l
ξl∑{Tk ,Dl}
1
where {T ,D} is the set of all CDT-D configurations and {Tk ,Dl}
is the set of CDT-D configs. with k triangles and l dimers.
I The radius of convergence of the power sum in g is it’scritical value denoted gc(ξ).
I At gc(ξ), the PF, Z (gc , ξ) behaves non-analytically.
I A critical point can be characterized by it’s Hausdorffdimension dH:
〈Area(R)〉∝RdH
Partition Function
The partition function (PF) of this model is the sum of theweight over all possible CDT-D configurations:
Z (g , ξ) =∑{T ,D}
gN(T )ξN(D) =∑
k
gk
∑l
ξl∑{Tk ,Dl}
1
where {T ,D} is the set of all CDT-D configurations and {Tk ,Dl}is the set of CDT-D configs. with k triangles and l dimers.
I The radius of convergence of the power sum in g is it’scritical value denoted gc(ξ).
I At gc(ξ), the PF, Z (gc , ξ) behaves non-analytically.
I A critical point can be characterized by it’s Hausdorffdimension dH:
〈Area(R)〉∝RdH
Partition Function
The partition function (PF) of this model is the sum of theweight over all possible CDT-D configurations:
Z (g , ξ) =∑{T ,D}
gN(T )ξN(D) =∑
k
gk
∑l
ξl∑{Tk ,Dl}
1
where {T ,D} is the set of all CDT-D configurations and {Tk ,Dl}
is the set of CDT-D configs. with k triangles and l dimers.
I The radius of convergence of the power sum in g is it’scritical value denoted gc(ξ).
I At gc(ξ), the PF, Z (gc , ξ) behaves non-analytically.
I A critical point can be characterized by it’s Hausdorffdimension dH:
〈Area(R)〉∝RdH
Partition Function
The partition function (PF) of this model is the sum of theweight over all possible CDT-D configurations:
Z (g , ξ) =∑{T ,D}
gN(T )ξN(D) =∑
k
gk
∑l
ξl∑{Tk ,Dl}
1
where {T ,D} is the set of all CDT-D configurations and {Tk ,Dl}
is the set of CDT-D configs. with k triangles and l dimers.
I The radius of convergence of the power sum in g is it’scritical value denoted gc(ξ).
I At gc(ξ), the PF, Z (gc , ξ) behaves non-analytically.
I A critical point can be characterized by it’s Hausdorffdimension dH:
〈Area(R)〉∝RdH
Partition Function
The partition function (PF) of this model is the sum of theweight over all possible CDT-D configurations:
Z (g , ξ) =∑{T ,D}
gN(T )ξN(D) =∑
k
gk
∑l
ξl∑{Tk ,Dl}
1
where {T ,D} is the set of all CDT-D configurations and {Tk ,Dl}
is the set of CDT-D configs. with k triangles and l dimers.
I The radius of convergence of the power sum in g is it’scritical value denoted gc(ξ).
I At gc(ξ), the PF, Z (gc , ξ) behaves non-analytically.
I A critical point can be characterized by it’s Hausdorffdimension dH:
〈Area(R)〉∝RdH
Partition Function
The partition function (PF) of this model is the sum of theweight over all possible CDT-D configurations:
Z (g , ξ) =∑{T ,D}
gN(T )ξN(D) =∑
k
gk
∑l
ξl∑{Tk ,Dl}
1
where {T ,D} is the set of all CDT-D configurations and {Tk ,Dl}
is the set of CDT-D configs. with k triangles and l dimers.
I The radius of convergence of the power sum in g is it’scritical value denoted gc(ξ).
I At gc(ξ), the PF, Z (gc , ξ) behaves non-analytically.
I A critical point can be characterized by it’s Hausdorffdimension dH:
〈Area(R)〉∝RdH
Labelled Trees
It was observed that CDT-D configurations have a bijection withlabelled trees (tree graphs with vertices carrying labels).
Figure: The tree that corresponds to a CDT-D configuration
Restricted Dimer Model
It turns out that these trees are non-local (i.e branches which donot share a root are nonetheless correlated).
I A ban on CDT-D configurations which are mapped tonon-local trees
I A ban on dimers falling across two backward triangles
Figure: Banned dimer type
In this restricted CDT-D model one can use the generatingfunctions of labelled trees to calculate Z (g , ξ).
Restricted Dimer Model
It turns out that these trees are non-local (i.e branches which donot share a root are nonetheless correlated).
I A ban on CDT-D configurations which are mapped tonon-local trees
I A ban on dimers falling across two backward triangles
Figure: Banned dimer type
In this restricted CDT-D model one can use the generatingfunctions of labelled trees to calculate Z (g , ξ).
Restricted Dimer Model
It turns out that these trees are non-local (i.e branches which donot share a root are nonetheless correlated).
I A ban on CDT-D configurations which are mapped tonon-local trees
I A ban on dimers falling across two backward triangles
Figure: Banned dimer type
In this restricted CDT-D model one can use the generatingfunctions of labelled trees to calculate Z (g , ξ).
Restricted Dimer Model
It turns out that these trees are non-local (i.e branches which donot share a root are nonetheless correlated).
I A ban on CDT-D configurations which are mapped tonon-local trees
I A ban on dimers falling across two backward triangles
Figure: Banned dimer type
In this restricted CDT-D model one can use the generatingfunctions of labelled trees to calculate Z (g , ξ).
A Summary of my work
There are 2 main things that I worked on and completed:
I Solving the un-restricted CDT-D model
I Finding the continuum propagator in the restricted CDT-Dmodel
A Summary of my work
There are 2 main things that I worked on and completed:
I Solving the un-restricted CDT-D model
I Finding the continuum propagator in the restricted CDT-Dmodel
A Summary of my work
There are 2 main things that I worked on and completed:
I Solving the un-restricted CDT-D model
I Finding the continuum propagator in the restricted CDT-Dmodel
The un-restricted dimer modelOne of the restrictions lifted was the ban on:
Figure: The now integrated dimer type
I One does not find any new critical points.
I The previously known result holds: there are values of ξ forwhich the PF has a cube-root singularity as g→gc withdH = 3 and 3/2 and others where the PF has a square-rootsingularity with dH = 2. The dH = 2 points corresponds topure CDT.
I Recently solved the model with the non-local trees too.Maybe this will have new critical points?
The un-restricted dimer modelOne of the restrictions lifted was the ban on:
Figure: The now integrated dimer type
I One does not find any new critical points.
I The previously known result holds: there are values of ξ forwhich the PF has a cube-root singularity as g→gc withdH = 3 and 3/2 and others where the PF has a square-rootsingularity with dH = 2. The dH = 2 points corresponds topure CDT.
I Recently solved the model with the non-local trees too.Maybe this will have new critical points?
The un-restricted dimer modelOne of the restrictions lifted was the ban on:
Figure: The now integrated dimer type
I One does not find any new critical points.
I The previously known result holds: there are values of ξ forwhich the PF has a cube-root singularity as g→gc
withdH = 3 and 3/2 and others where the PF has a square-rootsingularity with dH = 2. The dH = 2 points corresponds topure CDT.
I Recently solved the model with the non-local trees too.Maybe this will have new critical points?
The un-restricted dimer modelOne of the restrictions lifted was the ban on:
Figure: The now integrated dimer type
I One does not find any new critical points.
I The previously known result holds: there are values of ξ forwhich the PF has a cube-root singularity as g→gc withdH = 3 and 3/2
and others where the PF has a square-rootsingularity with dH = 2. The dH = 2 points corresponds topure CDT.
I Recently solved the model with the non-local trees too.Maybe this will have new critical points?
The un-restricted dimer modelOne of the restrictions lifted was the ban on:
Figure: The now integrated dimer type
I One does not find any new critical points.
I The previously known result holds: there are values of ξ forwhich the PF has a cube-root singularity as g→gc withdH = 3 and 3/2 and others where the PF has a square-rootsingularity with dH = 2.
The dH = 2 points corresponds topure CDT.
I Recently solved the model with the non-local trees too.Maybe this will have new critical points?
The un-restricted dimer modelOne of the restrictions lifted was the ban on:
Figure: The now integrated dimer type
I One does not find any new critical points.
I The previously known result holds: there are values of ξ forwhich the PF has a cube-root singularity as g→gc withdH = 3 and 3/2 and others where the PF has a square-rootsingularity with dH = 2. The dH = 2 points corresponds topure CDT.
I Recently solved the model with the non-local trees too.Maybe this will have new critical points?
The un-restricted dimer modelOne of the restrictions lifted was the ban on:
Figure: The now integrated dimer type
I One does not find any new critical points.
I The previously known result holds: there are values of ξ forwhich the PF has a cube-root singularity as g→gc withdH = 3 and 3/2 and others where the PF has a square-rootsingularity with dH = 2. The dH = 2 points corresponds topure CDT.
I Recently solved the model with the non-local trees too.Maybe this will have new critical points?
The Propagator
I The propagator, Gg ,ξ(l1, l2; t) is the transition amplitudefrom a loop of length l1 to one of length l2 in t time-steps.
I This can be calculated using the same labelled treetechniques
The Propagator
I The propagator, Gg ,ξ(l1, l2; t) is the transition amplitudefrom a loop of length l1 to one of length l2 in t time-steps.
I This can be calculated using the same labelled treetechniques
The Continuum limit
I We send a→ 0, keeping the physical time and boundarylengths, T := at; L1 := al1; L2 := al2 constant.
I Which means {t, l1, l2} → ∞, simultaneously.
I Hence, the weight of large graphs can’t be suppressed.
I So we must tune g to the radius of convergence gc(ξ) ofthe sum.
I The scaling behaviour of the approach to the critical value istaken to be (dH > 0):
g − gc ∝ adH Λ
I Λ: bulk cosmological constant.
I Finally the continuum propagator is obtained by:
GΛ(L1, L2;T ) = lima→0
aG(gc+adH Λ),ξ
(L1
a,L2
a;T
a
)
The Continuum limit
I We send a→ 0, keeping the physical time and boundarylengths, T := at; L1 := al1; L2 := al2 constant.
I Which means {t, l1, l2} → ∞, simultaneously.
I Hence, the weight of large graphs can’t be suppressed.
I So we must tune g to the radius of convergence gc(ξ) ofthe sum.
I The scaling behaviour of the approach to the critical value istaken to be (dH > 0):
g − gc ∝ adH Λ
I Λ: bulk cosmological constant.
I Finally the continuum propagator is obtained by:
GΛ(L1, L2;T ) = lima→0
aG(gc+adH Λ),ξ
(L1
a,L2
a;T
a
)
The Continuum limit
I We send a→ 0, keeping the physical time and boundarylengths, T := at; L1 := al1; L2 := al2 constant.
I Which means {t, l1, l2} → ∞, simultaneously.
I Hence, the weight of large graphs can’t be suppressed.
I So we must tune g to the radius of convergence gc(ξ) ofthe sum.
I The scaling behaviour of the approach to the critical value istaken to be (dH > 0):
g − gc ∝ adH Λ
I Λ: bulk cosmological constant.
I Finally the continuum propagator is obtained by:
GΛ(L1, L2;T ) = lima→0
aG(gc+adH Λ),ξ
(L1
a,L2
a;T
a
)
The Continuum limit
I We send a→ 0, keeping the physical time and boundarylengths, T := at; L1 := al1; L2 := al2 constant.
I Which means {t, l1, l2} → ∞, simultaneously.
I Hence, the weight of large graphs can’t be suppressed.
I So we must tune g to the radius of convergence gc(ξ) ofthe sum.
I The scaling behaviour of the approach to the critical value istaken to be (dH > 0):
g − gc ∝ adH Λ
I Λ: bulk cosmological constant.
I Finally the continuum propagator is obtained by:
GΛ(L1, L2;T ) = lima→0
aG(gc+adH Λ),ξ
(L1
a,L2
a;T
a
)
The Continuum limit
I We send a→ 0, keeping the physical time and boundarylengths, T := at; L1 := al1; L2 := al2 constant.
I Which means {t, l1, l2} → ∞, simultaneously.
I Hence, the weight of large graphs can’t be suppressed.
I So we must tune g to the radius of convergence gc(ξ) ofthe sum.
I The scaling behaviour of the approach to the critical value istaken to be (dH > 0):
g − gc ∝ adH Λ
I Λ: bulk cosmological constant.
I Finally the continuum propagator is obtained by:
GΛ(L1, L2;T ) = lima→0
aG(gc+adH Λ),ξ
(L1
a,L2
a;T
a
)
The Continuum limit
I We send a→ 0, keeping the physical time and boundarylengths, T := at; L1 := al1; L2 := al2 constant.
I Which means {t, l1, l2} → ∞, simultaneously.
I Hence, the weight of large graphs can’t be suppressed.
I So we must tune g to the radius of convergence gc(ξ) ofthe sum.
I The scaling behaviour of the approach to the critical value istaken to be (dH > 0):
g − gc ∝ adH Λ
I Λ: bulk cosmological constant.
I Finally the continuum propagator is obtained by:
GΛ(L1, L2;T ) = lima→0
aG(gc+adH Λ),ξ
(L1
a,L2
a;T
a
)
The Continuum limit
I We send a→ 0, keeping the physical time and boundarylengths, T := at; L1 := al1; L2 := al2 constant.
I Which means {t, l1, l2} → ∞, simultaneously.
I Hence, the weight of large graphs can’t be suppressed.
I So we must tune g to the radius of convergence gc(ξ) ofthe sum.
I The scaling behaviour of the approach to the critical value istaken to be (dH > 0):
g − gc ∝ adH Λ
I Λ: bulk cosmological constant.
I Finally the continuum propagator is obtained by:
GΛ(L1, L2;T ) = lima→0
aG(gc+adH Λ),ξ
(L1
a,L2
a;T
a
)
I Laplace transform in (L1, L2)→ (X,Y)
I GΛ(L1, L2;T )→ GΛ(X ,Y ;T )
I X and Y: boundary cosmological constants.
I Laplace transform in (L1, L2)→ (X,Y)
I GΛ(L1, L2;T )→ GΛ(X ,Y ;T )
I X and Y: boundary cosmological constants.
I Laplace transform in (L1, L2)→ (X,Y)
I GΛ(L1, L2;T )→ GΛ(X ,Y ;T )
I X and Y: boundary cosmological constants.
ResultsAround the critical point where dH = 3, the asymptotics of thecontinuum propagator is:
GΛ(X ,Y ,T →∞) =12Λ2/3e−
√3 3√ΛT
(√3 sin
(3√
ΛT)− cos
(3√
ΛT))
5(
3√
Λ + X)2 (
3√
Λ + Y)
GΛ(X ,Y ,T → 0) =2T
5
Laplace====⇒ 2T
5δ(L1)δ(L2)
The result from 2000 for the asymptotics of the continuumpropagator for pure CDT (the point with dH = 2) is:
GΛ(X ,Y ;T →∞) =4Λe−2
√ΛT
(√
Λ + X )2(√
Λ + Y )
GΛ(X ,Y ;T → 0) =1
X + Y
Laplace====⇒ δ(L1 − L2)
ResultsAround the critical point where dH = 3, the asymptotics of thecontinuum propagator is:
GΛ(X ,Y ,T →∞) =12Λ2/3e−
√3 3√ΛT
(√3 sin
(3√
ΛT)− cos
(3√
ΛT))
5(
3√
Λ + X)2 (
3√
Λ + Y)
GΛ(X ,Y ,T → 0) =2T
5
Laplace====⇒ 2T
5δ(L1)δ(L2)
The result from 2000 for the asymptotics of the continuumpropagator for pure CDT (the point with dH = 2) is:
GΛ(X ,Y ;T →∞) =4Λe−2
√ΛT
(√
Λ + X )2(√
Λ + Y )
GΛ(X ,Y ;T → 0) =1
X + Y
Laplace====⇒ δ(L1 − L2)
ResultsAround the critical point where dH = 3, the asymptotics of thecontinuum propagator is:
GΛ(X ,Y ,T →∞) =12Λ2/3e−
√3 3√ΛT
(√3 sin
(3√
ΛT)− cos
(3√
ΛT))
5(
3√
Λ + X)2 (
3√
Λ + Y)
GΛ(X ,Y ,T → 0) =2T
5
Laplace====⇒ 2T
5δ(L1)δ(L2)
The result from 2000 for the asymptotics of the continuumpropagator for pure CDT (the point with dH = 2) is:
GΛ(X ,Y ;T →∞) =4Λe−2
√ΛT
(√
Λ + X )2(√
Λ + Y )
GΛ(X ,Y ;T → 0) =1
X + Y
Laplace====⇒ δ(L1 − L2)
ResultsAround the critical point where dH = 3, the asymptotics of thecontinuum propagator is:
GΛ(X ,Y ,T →∞) =12Λ2/3e−
√3 3√ΛT
(√3 sin
(3√
ΛT)− cos
(3√
ΛT))
5(
3√
Λ + X)2 (
3√
Λ + Y)
GΛ(X ,Y ,T → 0) =2T
5
Laplace====⇒ 2T
5δ(L1)δ(L2)
The result from 2000 for the asymptotics of the continuumpropagator for pure CDT (the point with dH = 2) is:
GΛ(X ,Y ;T →∞) =4Λe−2
√ΛT
(√
Λ + X )2(√
Λ + Y )
GΛ(X ,Y ;T → 0) =1
X + Y
Laplace====⇒ δ(L1 − L2)